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Geometrical lattice engineering of complex oxide heterostructures: a designer approach to emergent quantum states

Published online by Cambridge University Press:  12 August 2016

Xiaoran Liu
Affiliation:
Department of Physics, University of Arkansas, Fayetteville, Arkansas 72701, USA
S. Middey
Affiliation:
Department of Physics, University of Arkansas, Fayetteville, Arkansas 72701, USA
Yanwei Cao
Affiliation:
Department of Physics, University of Arkansas, Fayetteville, Arkansas 72701, USA
M. Kareev
Affiliation:
Department of Physics, University of Arkansas, Fayetteville, Arkansas 72701, USA
J. Chakhalian*
Affiliation:
Department of Physics and Astronomy, Rutgers University, Piscataway, New Jersey 08854, USA
*
Address all correspondence to J. Chakhalian at [email protected]

Abstract

Epitaxial heterostructures composed of complex oxides have fascinated researchers for over a decade as they offer multiple degrees of freedom to unveil emergent many-body phenomena often unattainable in bulk. Recently, apart from stabilizing such artificial structures along the conventional [001]-direction, tuning the growth direction along unconventional crystallographic axes has been highlighted as a promising route to realize novel quantum many-body phases. Here we illustrate this rapidly developing field of geometrical lattice engineering with the emphasis on a few prototypical examples of the recent experimental efforts to design complex oxide heterostructures along the (111) orientation for quantum phase discovery and potential applications.

Type
Functional Oxides Prospective Article
Copyright
Copyright © Materials Research Society 2016 

Introduction

The search and exploration of new collective quantum states are of prime importance and interest in the condensed matter physics. Toward this goal, ultra-thin heterostructures composed of two or more structurally, chemically, and electronically dissimilar constituent oxides have been developed into a powerful approach over the past decade.[ Reference Chakhalian, Freeland, Millis, Panagopoulos and Rondinelli 1 Reference Poeppelmeier and Rondinelli 6 ] The main notion here is that at the interface where the dissimilarities meet, the frustration caused by mismatches between arrangement of atoms, charges, orbitals, or spins can trigger the emergence of phenomena with electronic and magnetic structures markedly different from the corresponding bulk compositions.[ Reference Chakhalian, Freeland, Millis, Panagopoulos and Rondinelli 1 ] As a result, the interface engineering (IE) has opened a route to novel material behaviors by means of those mismatches as the control parameters. The IE approach is intimately connected to another popular approach to tailor the properties of materials with epitaxial strain by effectively altering the bond-length and bond-angle of structural units through the deliberate choice of substrates. The exploration of epitaxial strain due to the lattice mismatch has been thus far successfully used to manipulate the electronic bandwidth, band filling, ferroelectric, and magnetic interactions of the ultra-thin films.[ Reference Liu, Kargarian, Kareev, Gray, Ryan, Cruz, Tahir, Chuang, Guo, Rondinelli, Freeland, Fiete and Chakhalian 7 Reference Chakhalian, Rondinelli, Liu, Gray, Kareev, Moon, Prasai, Cohn, Varela, Tung, Bedzyk, Altendorf, Strigari, Dabrowski, Tjeng, Ryan and Freeland 9 ]

Inspired by the success of those engineering methods, very recently another promising venue collectively known as geometrical lattice engineering (GLE) has been presented as a powerful tool to forge new topological and quantum many-body states.[ Reference Xiao, Zhu, Ran, Nagaosa and Okamoto 10 Reference Rüegg and Fiete 12 ] In close synergy with the IE and strain engineering (SE) where mismatches between layers can induce unusual interactions, the key idea behind the GLE is to design fully epitaxial ultra-thin heterostructures with an artificial lattice geometry generated by stacking of a very specific number of atomic planes along a specific orientation. This concept can be further illustrated by realizing that for a three-dimensional (3D) material the stacking of two-dimensional (2D) atomic planes, the specific arrangement of ions in those planes, their sequence, and the periodicity of layers fulfilling a complete unit cell can exhibit drastic variations depending on the crystallographic direction along which it is projected. Conventionally, for rather thick bulk-like films, the effect of those variations is often negligible (apart from anisotropy), whereas for the ultra-thin samples it becomes much more dominant in determining the electronic and magnetic properties. Following this idea, in the pursuit of exotic quantum states many interesting material systems have been proposed theoretically[ Reference Xiao, Zhu, Ran, Nagaosa and Okamoto 10 Reference Cai, Li, Wang, Ju, Feng and Gong 22 ], while the experimental work on GLE has been primarily focused on growth of cubic or pseudocubic (pc) (111)-oriented artificial lattices[ Reference Middey, Meyers, Kareev, Moon, Gray, Liu, Freeland and Chakhalian 23 Reference Panomsuwan, Takai and Saito 28 ].

The rest of the paper is organized as follows. First, we will illustrate the concept of GLE by describing several prototypical examples with (111) orientation to shed light on the details of their design, fabrication, and possible growth challenges. By no means does this paper present a comprehensive review of GLE. We have not attempted to review the large body of published results. Instead, we have focused on a few selected results to illustrate the concepts, methodologies, and physics behind the described phenomena. We apologize for possible omissions. In the final section, a brief outlook will be provided to accentuate some intriguing new ideas and material systems with other lattice orientations and highlight the significant but largely unexplored potential of GLE for quantum phase discovery and applications.

Control parameters of GLE

In general, the GLE concept is comprised of three controllable stages throughout the process of heteroepitaxial fabrication. Here, we use a 3D simple cubic unit-cell model to schematically illustrate these control parameters, as shown in Fig. 1.

  1. A. Growth orientation: Starting with the same bulk compound, its 3D crystal structure is viewed as a stacking of atomic layers with different in-plane lattice geometries along different directions. For example, as shown in Fig. 1, while the (001) planes have square symmetry, the (110) and (111) planes have rectangular and triangular geometries, respectively. The required in-plane lattice geometry by design can be thus determined by selecting the proper structure and orientation of the substrate surface, which acts as a guiding template during the initial stage of nucleation and growth. A typical example for this case is the realization of 2D magnetically frustrated lattices derived from ultra-thin (111)-oriented spinel-type structure AB 2O4 (for more details see section “Geometrically frustrated lattices”).

  2. B. Out-of-plane stacking sequence: In a bulk crystal, the periodicity of the atomic layers to fulfill the requirement of translational symmetry as well as the relative atomic positions in neighboring lattice planes vary dramatically with the specific choice of the crystallographic direction. For instance, the stacking of the adjacent layers can be either right on top of each other [the (001) stacking in Fig. 1], or shifted [the (110) stacking], or even entirely inversed [the (111) stacking]. This observation is of paramount importance for the design of artificial heterostructures since by controlling the number of stacking layers within that period one can devise unique quasi-2D lattices that cannot be obtained in the naturally formed crystals. Among the prominent example of GLE we cite the generalized graphene lattice, which can be obtained by digitally tuning the number of atomic layers of (111)-oriented ABO3 perovskite-type structures for searching potential topological phases with and without spin–orbit active ions (for more details see section “Generalized graphene lattice from ABO3 perovskites”).

  3. C. Isostructural superlattices approach: Combining isostructural materials together to establish superlattice structures via digital control over the individual number of layers adds another practical dimension to the application of GLE. This approach can be very useful for the purpose of achieving materials with complex chemical compositions or even thermodynamically unstable phases in the bulk form. A representative test case is the fabrication of (111)-oriented 1ABO3/1AB′O3 superlattices [here “1” refers to single pc/cubic unit cell], giving rise to A 2 BB′O6 double perovskite. Further examples can be found in section “Artificial double-perovskite lattice”.

Figure 1. Schematic illustration of the idea about geometrical lattice engineering, which has three control parameters named as orientation, stacking, and superlattice throughout its entire process.

In what follows, we discuss in some details how the control parameters of GLE can be experimentally realized in the fabrication of complex oxide thin films and superlattices.

Geometrically frustrated lattices

Various geometrically frustrated magnetic systems, including spin ice, spin glass, and spin liquid have been studied over several decades.[ Reference Mila 29 Reference Binder and Young 34 ] In such systems, the exchange interaction between nearest neighbor ions is typically antiferromagnetic (for spin ice, the exchange interaction is ferromagnetic) and the peculiar geometries of the lattices (triangular and kagome lattice for the 2D case, or pyrochlore and hyper-kagome lattice for the 3D case) render the magnetic bonds impossible to be satisfied simultaneously. These geometrically frustrated lattices, especially the 2D ones have an excellent potential to host various intriguing exotic phenomena such as quantum spin liquid, topological phases, kinetic ferromagnetism, and chiral superconducting state to list a few.[ Reference Han, Helton, Chu, Nocera, Rodriguez-Rivera, Broholm and Lee 16 , Reference Punk, Chowdhury and Sachdev 35 Reference Yu and Li 37 ] The fabrication of a 2D geometrically frustrated lattice, however, has proven to be rather challenging. For example, even though several metal–organic hybrid counterparts were synthesized by chemical methods, structural disorder, and strong lattice distortions remained a persistent hindrance.[ Reference Liu, Kravstsov, Beauchamp, Eubank and Eddaoudi 38 , Reference Nytko, Helton, Müller and Nocera 39 ] Alternatively, the GLE approach offers a promising way to generate such frustrated lattice by growing ultra-thin spinels along the [111] crystallographic axis, as shown in Fig. 2.

Figure 2. The conventional unit cell of a normal spinel structure. The corresponding (111) ionic planes are marked in the figures. Note, the A ionic planes only form the triangle planes, while the B ionic planes form both the triangle planes and also the kagome planes.

First we recap that the general chemical formula of the spinel structure can be written as A 1− δ Βδ [Α δ Β 2−δ ]O4; with δ = 0, it is known as normal spinel AB 2O4, in which all A-site cations are tetrahedrally coordinated, while all B-site cations are octahedrally coordinated. Next we point out that the normal spinel shows a structurally unique feature when viewed along the [111] crystallographic axis. Specifically, the crystal structure can be regarded as a stacking of alternative lattice planes, each of which is composed of single kind of ions (see Fig. 2). In this stacking, the O sublattice has the cubic close packing (CCP) atomic arrangement. In contrast, the A and B ionic planes show three distinct types of geometrically frustrated lattices: triangular A plane (T plane), triangular B plane (T′ plane), and kagome B plane (K plane) as displayed in Fig. 2. In the bulk, totally 18 ionic planes complete a full periodicity in the form of [OKOTT′–T]3 [ Reference Vaz, Henrich, Ann and Altman 40 ] with [OKOTT′–T] as the basic repeat unit. For the rest of this paper such a basic repeat unit is referred as “1 monolayer” of the (111)-oriented normal spinel.

From the synthesis point of view, there are two main issues one needs to overcome to obtain high-quality (111)-oriented normal spinel heterostructures. First, due to the limited availability of isostructural/isosymmetric substrates, large lattice mismatch (>5%) between the film and the substrate generally leads to incoherent or inhomogeneous growth. Secondly, a magnetically passive spacer in the superlattice has to be chemically stable and lattice symmetry compatible with the spinel structure. A complete solution to these issues has been recently demonstrated by Liu et al.[ Reference Liu, Choudhury, Cao, Middey, Kareev, Meyers, Kim, Ryan and Chakhalian 24 ] in the epitaxial growth of (111)-oriented CoCr2O4/Al2O3 (CCO/AlO) heterostructures. For this system, AlO was selected as both the substrate and spacer because: (1) AlO is a non-magnetic insulator with a large band gap of about 9 eV and (2) since along the (0001)-direction the oxygen sublattice consists of hexagonal close packing (HCP) arrangement, it has an in-plane lattice geometry, which almost perfectly matches the CCP arrangement of spinel [see Fig. 3(a)]. In addition, a fairly small lattice mismatch of ~3% can be obtained when we compare the respective in-plane O–O distances (AlO: 2.74 Å; CCO: 2.82 Å).

Figure 3. (111)-oriented CoCr2O4/Al2O3 (CCO/AlO) heterostructures. (a) Epitaxial relationship between CCO and AlO. The hexagonal close packing of AlO oxygen sublattice is labeled as AB in black, while the CCP of CCO oxygen sublattice is labeled as ABC in brown. (b)–(d) RHEED images during the growth of each component. The half-order reflections (marked by pink solid circles) observed on CCO layer is due to the double expansion of the in-plane unit cell. Reproduced from Ref. Reference Liu, Choudhury, Cao, Middey, Kareev, Meyers, Kim, Ryan and Chakhalian24, with the permission of AIP Publishing.

The spinel-based heterostructures were fabricated layer-by-layer using the pulsed laser deposition (PLD) technique. The structural properties of the resultant samples were characterized by X-ray reflectivity (XRR) and X-ray diffraction (XRD) measurements with the results for two prototypical samples [a thicker (2CCO/2AlO)10 and an ultra-thin (2CCO/1AlO)4] shown in Fig. 4. As seen, according to the XRR scans with fittings from Fig. 4(a), 1CCO has a thickness of ~4.93 Å, while 1AlO ~13.5 Å and the average interface roughness is about 3 Å. On the other hand, the XRD 2θω scans shown in Fig. 4(b) in the vicinity of the substrate (006) reflection confirm that the films are grown along the (111)-direction with no additional peaks from impurity phase. In particular, besides the film's (222) main reflection (labeled as 0th), the superlattice's satellite peaks labeled as ±1st were clearly distinguishable and the number of the thickness fringes between the main peak and the satellite peak agrees quite well with the superlattice repeat pattern. These observations provide a solid evidence that growth of the geometrically engineered spinel-type structures along (111) is experimentally feasible.

Figure 4. (a) X-ray reflectivity and (b) x-ray diffraction curves of 2CCO/nAlO (n = 1 and 2) superlattices. Both the thickness fringes and the superlattice satellite peaks are clearly seen from the graphs. (c, d) x-ray absorption spectra of the CCO/AlO superlattices on the L 2,3 edges of Co and Cr, respectively. The spectra of CCO powders with normal spinel structure are plotted as references [Figs4(a) and 4(b) adapted with permission of AIP Publishing from Ref. Reference Chopdekar, Liberati, Takamura, Kourkoutis, Bettinger, Nelson-Cheeseman, Arenholz, Doran, Scholl, Muller and Suzuki46].

Another important issue is related to cation disorder or a mixture of various cation valences that can occur during the growth of spinel films[ Reference Liu, Kareev, Cao, Liu, Middey, Meyers, Freeland and Chakhalian 41 Reference Chopdekar, Liberati, Takamura, Kourkoutis, Bettinger, Nelson-Cheeseman, Arenholz, Doran, Scholl, Muller and Suzuki 46 ] and if present it may potentially destroy the expected normal spinel stacking patterns. Thus, it was necessary to investigate the chemical states and environments of both Co and Cr ions in the films. Such information can be readily probed by soft x-ray absorption spectroscopy (XAS) measurements. This synchrotron-based technique is extremely sensitive to the local electronic properties of a specific chemical element. The dataset was collected on the L 3,2 absorption edge of both Co and Cr elements of a representative 2CCO/2AlO superlattice in the total electron yield. As seen in Figs. 4(c) and 4(d), both the Co and Cr XAS of the 2CCO/2AlO sample have lineshapes (including the peak positions as well as the fine multiplet features) almost identical to those of the CCO bulk samples implying the absence of any detectable cation distribution disorder or mixture of chemical valences. This result further confirmed that the normal spinel structure was indeed maintained in the superlattice (i.e., Co2+ ions were tetrahedrally coordinated, while Cr3+ ions were octahedrally coordinated).

It is worth noting that in addition to sandwiching the ultrathin spinel structure toward 2D limit with magnetically inactive spacers[ Reference Liu, Choudhury, Cao, Middey, Kareev, Meyers, Kim, Ryan and Chakhalian 24 , Reference Yahiro, Tanaka, Yamamoto and Kawai 47 ], it may be also interesting to explore (111)-oriented all magnetic spinel superlattices. To illustrate this idea we note that since magnetic properties of spinels strongly depend on the exchange interaction between A and B sites, the periodic modulation of the exchange interaction in artificial superlattices can give rise to novel properties not existing in either the single composition or the solid solution. Murata et al.[ Reference Murata, Kozuka, Uchida and Kawasaki 48 ] recently reported the growth of such ZnFe2O4/ZnCr2O4 superlattices on MgAl2O4 (111) substrates. Both of the constituent layers have a normal spinel structure with non-magnetic A sites (Zn2+, S = 0) and magnetic B sites (Fe3+, S = 5/2; Cr3+, S = 3/2). The effect of GLE was investigated by measuring zero field cooling (ZFC) and field cooling (FC) magnetic susceptibilities of the ZnFe2O4 and the ZnCr2O4 thin films, the Zn(CrFe)O4 solid solution, and the mZnFe2O4/mZnCr2O4 (m = 1, 2, 4, and 10) superlattices. In the bulk, both materials are characterized by large and negative Curie–Weiss temperatures; the ZnFe2O4 film shows spin–glass behavior below ~17 K, while ZnCr2O4 film shows antiferromagnetic ordering below 13 K. In contrast to this, the Zn(CrFe)O4 solid solution exhibits a distinct spin–glass behavior below 28 K. This higher transition temperature T g is attributed to the random distributions of the Fe3+ and Cr3+ ions on the B sites causing spatially inhomogeneous exchange interactions. On the other hand, the spin–glass behavior was also observed for all of the superlattice films with a non-monotonic variation of T g with the layer thickness m. These experimental results were interpreted as the result of a periodic modulation of the exchange coupling between the B site ions across the interfaces. As the thickness of both layers becomes smaller, the number of the bulk-like Cr3+–O–Cr3+ as well as the Fe3+–O–Fe3+ magnetic bonds decreases. At the same time, more ZnFe2O4/ZnCr2O4 interfaces appear where artificially induced antiferromagnetic Cr3+–O–Fe3+ interaction starts to compete with the bulk-like magnetic interactions. As the result of such competition, the formation of a long-range magnetic ordering is suppressed and the spin–glass behavior gradually arises. In addition, once the layer thickness of each composition decreases below a certain critical limit (m = 4), the material can be viewed as mainly being made of the interfaces where the induced Cr3+–O–Fe3+ interaction is dominant and a new magnetic state dramatically different from the bulk appears in the superlattice. The suppression of the spin–glass behavior for 1 < m < 4 was interpreted originating from some new type of short-range magnetic clusters induced by the Cr3+–O–Fe3+ interaction, which again does not exist in the constituent bulk compounds. These examples corroborate that apart from chemical doping and epitaxial strain, GLE of the stacking layers as well as their sequences in the heterostructures is an effective way to alter electronic and magnetic behaviors.

Generalized graphene lattice from ABO3 perovskites

Perovskite oxides are the host of diverse properties including metal–insulator transition, magnetism, superconductivity, charge, and orbital orderings, multiferroicity, etc. These infinite layer ABO3 perovskite compounds consist of alternating AO/BO2, ABO/O2, and AO3/B atomic planes along the pc [001], [110], and [111] directions, respectively. Thus, the precise control during the growth of two or three pc unit cells of ABO3 along the (111) orientation leads to new lattice geometries with vertically shifted triangular planes of B sites and results in buckled honeycomb lattice[ Reference Xiao, Zhu, Ran, Nagaosa and Okamoto 10 Reference Rüegg and Fiete 12 ] and dice lattice[ Reference Wang and Ran 49 ] respectively as shown in Fig. 5. The emergence of striking topological phases including anomalous quantum Hall state was originally predicted in a honeycomb lattice by Haldane[ Reference Haldane 50 ], and recently initiated active searches for artificially stabilized graphene like quasi-2D lattice that can provide an ideal playground for interacting topological phases in complex oxides[ Reference Xiao, Zhu, Ran, Nagaosa and Okamoto 10 Reference Rüegg and Fiete 12 , Reference Wang, Wang, Fang and Dai 14 , Reference Okamoto 19 Reference Lado, Pardo and Baldomir 21 , Reference Rüegg, Mitra, Demkov and Fiete 51 Reference Okamoto, Zhu, Nomura, Arita, Xiao and Nagaosa 59 ]. Here we describe the case of rare-earth nickelates that vividly illustrates the opportunities for designer topological phases by GLE.

Figure 5. Buckled honeycomb lattice and Dice lattice geometry can be generated by epitaxial growth of perovskite system along the [111] direction. A sites are not shown for Dice lattice due to visual clarity.

The first member of rare earth nickelates series, LaNiO3 is a paramagnetic metal. The other members (RENiO3 with RE = Pr, Nd,…,Lu, and Y) in the bulk form exhibit metal–insulator transition, E′-type antiferromagnetic ordering, charge ordering and structural transition with a strong dependence of the transition temperature on the size of RE ions[ Reference Medarde 60 , Reference Catalan 61 ]. The possibility of realizing cuprate-like Fermi surface has led to a rapid development and study of (001)-oriented ultra-thin films and superlattices of various members of the RENiO3 family (see Ref. [Reference Middey, Chakhalian, Mahadevan, Freeland, Millis and Sarma62] for review). Several theoretical works[ Reference Yang, Zhu, Xiao, Okamoto, Wang and Ran 11 , Reference Rüegg and Fiete 12 , Reference Rüegg, Mitra, Demkov and Fiete 51 Reference Doennig, Pickett and Pentcheva 53 ] further emphasized the possibility of realizing interaction-driven topological phases without spin-orbit (e.g., Dirac half semimetal phase, quantum anomalous Hall insulator phase, or ferromagnetic nematic phase) in the weakly correlated limit on the buckled honeycomb lattice of RENiO3. Moreover, in contrast to the bulk LaNiO3, where orbital ordering is not present, theoretical modeling in strongly correlated limit predicted the presence of an orbitally ordered magnetic phase as the ground state[ Reference Rüegg and Fiete 12 , Reference Rüegg, Mitra, Demkov and Fiete 51 Reference Doennig, Pickett and Pentcheva 53 ] for the buckled honeycomb lattice of LaNiO3.

Despite the conceptual simplicity, growth of perovskites along the [111]-direction presents formidable challenge. Contrary to the [001]pc-direction, the epitaxial stabilization along [111]pc direction is far less explored due to unavoidable surface/chemical reconstruction effects as all perovskite substrates are strongly polar along this direction, e.g., SrTiO3: [SrO3]4−, Ti4+; LaAlO3:[LaO3]3−, Al3+, and so on. While growing a metallic buffer layer at the very beginning of growth may help to avoid this polarity problem by effective screening of dipoles[ Reference Blok, Wan, Koster, Blank and Rijnders 63 ], one should pay particular attention as unwanted interfacial (between buffer layer and desired material) effects may have significant influence on the buffered heterostructure. As the reconstruction effect often appears only at the substrate–vacuum interface, the choice of a substrate with the same charge per plane sequence as that of the desired material can be another solution to this problem, which does not require to grow a buffer layer. To investigate this, Middey et al.[ Reference Middey, Rivero, Meyers, Kareev, Liu, Cao, Freeland, Barraza-Lopez and Chakhalian 64 ] have grown LaNiO3 films on SrTiO3 [with polar jump at film/substrate interface: see the upper panel of Fig. 6(a)] and LaAlO3 [without any polar jump at film/substrate interface: see lower panel of Fig. 6(a)] (111) substrate using pulsed laser interval deposition. The growth was monitored by in situ high-pressure reflection high-energy electron diffraction (RHEED). It was shown that while thick bulk-like LaNiO3 film is metallic and can effectively screen charge dipoles, a few unit-cell thin LNO film is insulating because of quantum confinement[ Reference Middey, Meyers, Kareev, Moon, Gray, Liu, Freeland and Chakhalian 23 ], and does require additional effects to avoid polar catastrophe. Specifically, in sharp contrast to the film grown on LAO (111), the presence of additional Bragg reflections [inset in Fig. 6(b)] for the 5 uc film on STO (111) confirmed the appearance of an additional non-perovskite phase during the initial stage of LNO growth. This secondary chemical phase was identified as La2Ni2O5 from the XRD, which was further corroborated by the observation of dominant contribution from Ni2+ ions in XAS spectrum [Fig. 6(b)]. Similar secondary phase formation has been also reported for the LNO film on STO (111), grown by molecular beam epitaxy[ Reference Freeland, Tung, Luo, Zhou, Lee, Chang, Morgan, Bedzyk and Fong 65 ]. With the increase of LNO film thickness, the increased metallicity screens the effect of polar jump and the relative amount of Ni3+ ions increases for the expense of Ni2+. Finally, stoichiometric LaNiO3 along [111] was obtained at about 15 uc. On the other hand, Ni3+ was stabilized from the very initial stage of growth of LNO on the LAO (111) substrate and thus confirmed that the absence of a polar jump at the film/substrate interface was critically important for the epitaxial stabilization along [111]. As a result, the desired generalized graphene-like crystal of RENiO3 with RE = La to Nd was successfully achieved on the LAO (111) substrate[ Reference Middey, Meyers, Kareev, Moon, Gray, Liu, Freeland and Chakhalian 23 ].

Figure 6. (a) Schematics (assuming pure ionic picture) to demonstrate the presence (absence) of polar jump for RENiO3 on SrTiO3 (LaAlO3) (111) substrate[ Reference Catalan 61 ]. (b) XAS of 5 uc LNO films on LAO and STO (111) have been compared with bulk Ni2+O, and LaNi3+O3. RHEED pattern of these films, recorded along pc [1−1 0]. For details, see Ref. Reference Blok, Wan, Koster, Blank and Rijnders63. (c) Experimental arrangement for measuring XLD of (111)-oriented superlattice (upper panel) and XA spectra recorded for a [2NdNiO3/4LaAlO3]×3 SL grown on LAO (111) using vertically (V) and horizontally (H) polarized x-ray and their difference are plotted in lower panel. Due to strong overlap of Ni L 3 edge with La M 4 edge (from the substrate and spacer layer LAO), only Ni L 2 edge is shown. Panel(c) adapted with permission from Ref. Reference Middey, Meyers, Doennig, Kareev, Liu, Cao, Yang, Shi, Gu, Ryan, Pentcheva, Freeland and Chakhalian25. Copyrighted by the American Physics Society.

According to the theoretical calculations[ Reference Rüegg and Fiete 12 , Reference Rüegg, Mitra, Demkov and Fiete 51 ], the QAH topological phases should be accompanied by spontaneous ferromagnetism. X-ray resonant magnetic scattering measurements on 2NdNiO3/4LaAlO3 (111) (denoted as 2NNO/4LAO) superlattice, however, ruled out the possibility of a long-range ferromagnetic ground state and instead established the presence of antiferromagnetic correlations. In addition, XAS measurements using linearly polarized x-rays found the presence of large (about 9%) X-ray linear dichroism (XLD) on Ni L 2 edge, as shown in Fig. 6(c). This XLD signal together with the ab intio calculations concludes an unusual antiferro-orbital-ordered state, which does not exist in either bulk or (001)-oriented nickelate thin films or heterostructures[ Reference Middey, Meyers, Doennig, Kareev, Liu, Cao, Yang, Shi, Gu, Ryan, Pentcheva, Freeland and Chakhalian 25 ]. In short, the artificially stabilized buckled honeycomb lattice structure for various other perovskite-based transition metal oxides can be a very promising route for realizing new types of correlated Mott phases or interacting topological phases. In addition, very recently the fabrications of (111)-oriented bilayers and trilayers of transition metal perovskites SrIrO3 have been reported[ Reference Hirai, Matsuno and Takagi 26 , Reference Anderson, Ryu, Zhou, Xie, Podkaminer, Ma, Irwin, Pan, Rzchowski and Eom 27 ] with the goal to access new topological phases.

Another interesting application of GLE is connected to designer magnetic phases by layering along [111]. For example, LNO has been heterostructured with LaMnO3 (LMO) along the [111]-direction[ Reference Gibert, Zubko, Scherwitzl, Íñiguez and Triscone 66 ]. Although bulk LNO is paramagnetic and bulk LMO is antiferromagnetic, the (111)-oriented LNO/LMO superlattices found to exhibit strong exchange bias (EB) effect. We note that EB is generally observed for ferromagnetic/antiferromagnetic or ferromagnetic/spin–glass interface.[ Reference Nogués, Sort, Langlais, Skumryev, Suriñach, Muñoz and Baró 67 , Reference Ali, Adie, Marrows, Greig, Hickey and Stamps 68 ] This surprising result was attributed to the quantum confinement effect[ Reference Dong and Dagotto 69 ] and charge transfer between Ni and Mn[ Reference Lee and Han 70 ], which are more effective for (111) orientation compared with (001). Very recent XAS experiments confirmed the larger electron transfer across the interface for (111) heterostructures.[ Reference Piamonteze, Gibert, Heidler, Dreiser, Rusponi, Brune, Triscone, Nolting and Staub 71 ].

Artificial double-perovskite lattice

In the past decade, ordered double-perovskite oxides with the chemical formula A 2 BB′O6 (A is an alkali-earth ion, and B and B′ are two different transition metal ions) have motivated plethora of research activities.[ Reference Anderson, Greenwood, Taylor and Poeppelmeier 72 ] In this family, the B and B′ ions are naturally ordered by forming a rock salt sublattice with B–O–B′ super-exchange that can generate rich magnetic and topological behaviors depending on the choice of the transition metal elements. Thus, the ordered double perovskites offer an excellent engineering playground for which potential functionalities can be predicted and explored[ Reference Anderson, Greenwood, Taylor and Poeppelmeier 72 Reference Serrate, De Teresa and Ibarra 76 ]. From the synthesis perspective, in the bulk the formation of an ordered double perovskite requires a relatively large difference between the chemical valences of B and B′ ions. Moreover, the ionic radii difference between those ions must be within a limited range often preventing synthesis of a variety interesting structures.[ Reference Anderson, Greenwood, Taylor and Poeppelmeier 72 ] Consequently, there are formidable challenges for the bulk synthesis of many theoretically proposed ordered double-perovskite materials, which are expected to host many interesting phenomena[ Reference Cook and Paramekanti 20 , Reference Zhang, Huang, Haule and Vanderbilt 77 Reference Liu, Fuh and Wang 79 ]

With the recent advances in thin-film growth techniques, it was noticed that there is another way to overcome those limitations.[ Reference Gibert, Zubko, Scherwitzl, Íñiguez and Triscone 66 , Reference Ichikawa, Arai, Imai, Hagiwara, Sakama, Azuma, Shimakawa, Takano, Kotaka, Yonetani, Fujisawa, Shimizu, Ishikawa and Cho 80 Reference Chang, Lee, Jun, Kwon, Kim and Kim 83 ] As illustrated in Fig. 7, the structure of an ordered double-perovskite A 2 BB′O6 consists of alternating monolayers of ABO3 and AB′O3 placed along the (111) orientation. By epitaxially growing (111)-oriented 1ABO3/1AB′O3 superlattices, it is now possible to design a wide range of ordered double-perovskite compounds that have never been realized through traditional bulk synthesis. In contrast to the artificial graphene-like lattices, here the out-of-plane stacking sequence of each perovskite composition has to be maintained with a monolayer precision to realize the required double-perovskite structure.

Figure 7. B-site ordered double perovskites viewed along the conventional (001) and the unconventional (111) direction, respectively. The (001) rock-salt arrangement of the B and B′ sites is equivalent to (111) BO6 and B′O6 superlattice.

Following this idea, a series of artificial double-perovskite La2 BB′O6 (B and B′ = Fe, Cr, Mn, and Ni) in the thin film form were obtained by PLD[ Reference Gibert, Zubko, Scherwitzl, Íñiguez and Triscone 66 , Reference Ueda, Tabata and Kawai 81 , Reference Ueda, Tabata and Kawai 82 ]. Among these materials, the artificial La2FeCrO6 (1LaFeO3–1LaCrO3) system has been extensively investigated and yet some controversy about its electronic and magnetic structure remained due to complexity of Fe3+–O–Cr3+ superexchange.[ Reference Kanamori 84 ]. Ueda et al.[ Reference Ueda, Tabata and Kawai 81 ] grew the artificial La2FeCrO6 (LFCO) films for the first time and found the samples to show ferromagnetic behavior. However, the small magnetic moment of only ~0.009 µ B at 0.1 T raised questions about the true nature of the magnetic ordering; to complicate the case both canted antiferromagnetic and ferrimagnetic ground states have been theoretically predicted.[ Reference Pickett 85 ]

To resolve the controversy, Gray et al.[ Reference Gray, Lee, Liu, Chakhalian and Freeland 86 ] synthesized artificial La2FeCrO6 and performed XAS and X-ray magnetic circular dichroism (XMCD) measurements at the L-edge of both Fe and Cr ions to probe the electronic and magnetic properties of each transition metal element. The corresponding absorption data shown in Fig. 8 confirmed that in the artificial LFCO compound both Fe and Cr are trivalent with high-spin configurations (Fe3+, S = 5/2; Cr3+, S = 3/2). In addition, the XMCD spectra of both elements revealed that the magnetic moments of Fe3+ and Cr3+ ions are parallel to each other. The estimated magnetic moments were about 0.3 µ B/Cr and 0.2 µ B/Fe at 5 T and appeared to be much smaller than the expected saturated values (3 µ B/Cr and 5 µ B/Fe). Furthermore, no detectable XMCD signal was observed for either ion under 0.1 T. Based on those observations, the artificial La2FeCrO6 was claimed to have a canted AFM ground state. Chakraverty et al.[ Reference Chakraveerty, Ohtomo, Okuyama, Saito, Okude, Kumai, Arima, Tokura, Tsukimoto, Ikuhara and Kawasaki 87 ] studied the relation between the degree of B-site disorder and the corresponding magnetic state on a series of thick LFCO films (up to a few hundred nanometers) that were synthesized with a LFCO polycrystalline target. They observed that only the high-quality B-site ordered sample show the expected saturated magnetization of ~2 µ B per LFCO formula, consistent with a ferrimagnetic ordering picture in which the local spin moment of Cr and Fe ions are anti-aligned, while the samples with sizable B, B′-site cation disorder show strong suppression of the total magnetic moment.

Figure 8. XAS and XMCD spectra on the L edge of (a) Fe and (b) Cr of the (111)-oriented 1LaFeO3/1LaCrO3 superlattice. Both spectra were measured at 10 K with an external magnetic field ~5 T applied parallel to the film surface. Data were collected in the total electron yield mode. Adapted from Ref. Reference Gray, Lee, Liu, Chakhalian and Freeland86, with the permission of AIP Publishing.

In addition, 1BiFeO3/1BiCrO3 (BFCO) artificial double-perovskite superlattice was also developed by Ichikawa et al.[ Reference Ichikawa, Arai, Imai, Hagiwara, Sakama, Azuma, Shimakawa, Takano, Kotaka, Yonetani, Fujisawa, Shimizu, Ishikawa and Cho 80 ] on STO (111) substrate and room temperature multiferroic behavior was observed on this system. Interestingly, the saturated magnetic moment per formula unit of the superlattice was much stronger than the signal of the film grown from the BFCO sputtering target[ Reference Nechache, Carignan, Gunawan, Harnagea, Botton and Menard 88 ]. This enhanced magnetization due to GLE sheds additional light on its potential for the development of new magnetic materials for application.

Summary and outlook

In the previous sections, the current status of GLE is discussed mainly with emphasis on the system layered along the cubic (or pc) (111) orientation of perovskites and spinels. However, the GLE concept is certainly not restricted to those systems and its realization opens wide opportunities for experimentalists to fabricate other interesting lattices in the heterostructured form. For instance, apart from spinel-type compounds, 2D frustrated lattices also appear in ultra-thin (111)-oriented pyrochlore (chemical formula: A 2 B 2O7) structures (Fig. 9, right panel on the top). This can be easily understood since the B sublattice in the pyrochlore structure is identical to that of spinel. Several theoretical works[ Reference Rüegg and Fiete 12 , Reference Guo and Franz 17 , Reference Hu, Zhong and Fiete 18 , Reference Yang and Nagaosa 89 ] have predicted the emergence of topological states with different B cations, while the experimental work on fabricating (111) pyrochlore films have been recently initiated[ Reference Fujita, Kozuka, Uchida, Tsukazaki, Arima and Kawasaki 90 Reference Chu, Riggs, Shapiro, Liu, Serero, Yi, Melissa, Suresha, Frontera, Vishwanath, Marti, Fisher and Ramesh 93 ]. Additionally, it was theoretically proposed that a monolayer of corundum-type (chemical formula: M2O3) structure grown along the (0001) direction could also form the graphene-like honeycomb lattice geometry[ Reference Afonso and Pardo 94 ] analogous to the perovskite (111) bilayers (Fig. 9, left panel on the top).

Figure 9. Summary and outlook on GLE. The upper panel displays other possible routines to topological phase and frustrated magnetism by applying pure GLE. The bottom panel presents the combination of GLE with IE or SE to establish new systems with intriguing physics such as quasi-particle excitation and emergent phenomena.

To push this field further, one can envision that a combination of GLE with other engineering approaches should allow for even more exotic phases. A fusion of GLE and IE may enable new tailor-made phenomena since for heterostructures the mismatches at the interface should be profoundly altered by the epitaxial orientation. For instance, while the basic scenario of two-dimensional electron gas (2DEG) at the interface between two insulating complex oxides has been interpreted within the “polar discontinuity” model[ Reference Ohtomo and Hwang 95 , Reference Nakagawa, Hwang and Muller 96 ], the polar mismatch patterns vary with the orientation of the heterostructure. This can be utilized to tune the carrier density and mobility of the 2DEG. Toward experimental realization of this idea a pioneering work has been reported on the growth of the prototypical LaAlO3/SrTiO3 system with (001), (110), and (111) interfaces (Fig. 9, right panel on the bottom)[ Reference Herranz, Sánchez, Dix, Scigaj and Fontcuberta 97 ]. Another interesting theory proposal is the study on the interface between (100)-oriented high-temperature superconducting cuprate YBa2Cu3O7 (YBCO) and colossal magnetoresistance manganite La x Ca1−x MnO3 (LCMO).[ Reference Takei, Fregoso, Galitski and Sarma 98 ] Compared to the extensively investigated (001) YBCO/LCMO interface[ Reference Chakhalian, Freeland, Habermeier, Cristiani, Khaliullin, van Veenendaal and Keimer 99 ] where the nodes of Cu d x2–y2 orbital are in the ab plane, the (100)-oriented YBCO has nodes of the d x2–y2 orbital out of the CuO2 plane (see Fig. 9, left panel on the bottom). This unique orbital coupling pattern is crucial for the emergence of exotic Majorana states[ Reference Catalano, Gibert, Bisogni, He, Sutarto, Viret, Zubko, Scherwitzl, Sawatzky, Schmitt and Triscone 100 ]. Furthermore, the combination of GLE and SE may open another interesting dimension for controlled modifications of the bond-length and bond-angle in structural units by epitaxial strain along the unconventional crystallographic axes.[ Reference Catalano, Gibert, Bisogni, He, Sutarto, Viret, Zubko, Scherwitzl, Sawatzky, Schmitt and Triscone 100 Reference Kim, Puggioni, Yuan, Xie, Zhou, Campbell, Ryan, Choi, Kim, Patzner, Ryu, Podkaminer, Irwin, Ma, Fennie, Rzchowski, Pan, Gopalan, Rondinelli and Eom 102 ]

To summarize, with the modern state-of-the-art thin-film fabrication methods, the notion of GLE can be experimentally realized and used as another control knob. Despite the challenges of layering with atomic precision along unconventional crystallographic directions, GLE has excellent potential for the discovery of novel electronic, magnetic, and topological phases with complex oxides.

Acknowledgments

The authors would like to thank D. Khomskii and G. Fiete for enlightening discussions. J.C. was supported by the Gordon and Betty Moore Foundation's EPiQS Initiative through Grant No. GBMF4534. X.L. and S.M. were supported by the Department of Energy under Grant No. DE-SC0012375, and Y.C. and M.K. were supported by the DOD-ARO under Grant No. 0402–17291.

References

1. Chakhalian, J., Freeland, J.W., Millis, A.J., Panagopoulos, C., and Rondinelli, J.M.: Colloquium: Emergent properties in plane view: strong correlations at oxide interfaces. Rev. Mod. Phys. 86, 1189 (2014).Google Scholar
2. Hwang, H.Y., Iwasa, Y., Kawasaki, M., Keimer, B., Nagaosa, N., and Tokura, Y.: Emergent phenomena at oxide interfaces. Nat. Mater. 11, 103 (2012).CrossRefGoogle ScholarPubMed
3. Chakhalian, J., Millis, A.J., and Rondinelli, J.: Whither the oxide interface. Nat. Mater. 11, 92 (2012).Google Scholar
4. Zubko, P., Gariglio, S., Gabay, M., Ghosez, P., and Triscone, J-M.: Interface physics in complex oxide heterostructures. Annu. Rev. Condens. Matter Phys. 2, 141 (2011).CrossRefGoogle Scholar
5. Stemmer, S. and Allen, S.J.: Two-dimensional electron gases at complex oxide interfaces. Annu. Rev. Mater. Res. 44, 151 (2014).Google Scholar
6. Poeppelmeier, K.R., and Rondinelli, J.M.: Oxide interfaces: mismatched lattices patched up. Nat. Chem. 8, 292 (2016).Google Scholar
7. Liu, J., Kargarian, M., Kareev, M., Gray, B., Ryan, P.J., Cruz, A., Tahir, N., Chuang, Y-D., Guo, J., Rondinelli, J.M., Freeland, J.W., Fiete, G.A., and Chakhalian, J.: Heterointerface engineered electronic and magnetic phases of NdNiO3 thin films. Nat. Commun. 4, 2714 (2013).Google Scholar
8. Choi, K.J., Biegalski, M., Li, Y.L., Sharan, A., Schubert, J., Uecker, R., Reiche, P., Chen, Y.B., Pan, X.Q., Gopalan, V., Chen, L.-Q., Schlom, D.G., and Eom, C.B.: Enhancement of ferroelectricity in strained BaTiO3 thin films. Science 306, 1005 (2004).Google Scholar
9. Chakhalian, J., Rondinelli, J.M., Liu, J., Gray, B.A., Kareev, M., Moon, E.J., Prasai, N., Cohn, J.L., Varela, M., Tung, I.C., Bedzyk, M.J., Altendorf, S.G., Strigari, F., Dabrowski, B., Tjeng, L.H., Ryan, P.J., and Freeland, J.W.: Asymmetric orbital–lattice interactions in ultrathin correlated oxide films. Phys. Rev. Lett. 107, 116805 (2011).Google Scholar
10. Xiao, D., Zhu, W., Ran, Y., Nagaosa, N., and Okamoto, S.: Interface engineering of quantum Hall effects in digital transition metal oxide heterostructures. Nat. Commun. 2, 596 (2011).Google Scholar
11. Yang, K., Zhu, W., Xiao, D., Okamoto, S., Wang, Z., and Ran, Y.: Possible interaction-driven topological phases in (111) bilayers of LaNiO3 . Phys. Rev. B 84, 201104(R) (2011).Google Scholar
12. Rüegg, A. and Fiete, G.A.: Topological insulators from complex orbital order in transition-metal oxides heterostructures. Phys. Rev. B 84, 201103(R) (2011).Google Scholar
13. Hu, X., Rüegg, A., and Fiete, G.A.: Topological phases in layered pyrochlore oxide thin films along the [111] direction. Phys. Rev. B 86, 235141 (2012).CrossRefGoogle Scholar
14. Wang, Y., Wang, Z., Fang, Z., and Dai, X.: Interaction-induced quantum anomalous Hall phase in (111) bilayer of LaCoO3 . Phys. Rev. B 91, 125139 (2015).CrossRefGoogle Scholar
15. Guo, H.M. and Franz, M.: Topological insulator on the kagome lattice. Phys. Rev. B 80, 113102 (2009).Google Scholar
16. Han, T., Helton, J.S., Chu, S., Nocera, D.G., Rodriguez-Rivera, J.A., Broholm, C., and Lee, Y.S.: Fractionalized excitations in the spin-liquid state of a kagome-lattice antiferromagnet. Nature 492, 406 (2012).CrossRefGoogle ScholarPubMed
17. Guo, H.-M. and Franz, M.: Three-dimensional topological insulators on the pyrochlore lattice. Phys. Rev. Lett. 103, 206805 (2009).CrossRefGoogle ScholarPubMed
18. Hu, X., Zhong, Z., and Fiete, G.A.: First principles prediction of topological phases in thin films of pyrochlore iridates. Sci. Rep. 5, 11072 (2015).CrossRefGoogle ScholarPubMed
19. Okamoto, S.: Doped Mott insulators in (111) bilayers of perovskite transition-metal oxides with a strong spin-orbit coupling. Phys. Rev. Lett. 110, 066403 (2013).Google Scholar
20. Cook, A.M. and Paramekanti, A.: Double perovskite heterostructures: magnetism, Chern bands and Chern insulators. Phys. Rev. Lett. 113, 077203 (2014).Google Scholar
21. Lado, J.L., Pardo, V., and Baldomir, D.: Ab initio study of Z2 topological phases in perovskite (111) (SrTiO3)7/(SrIrO3)2 and (KTaO3)7/(KPtO3)2 multilayers. Phys. Rev. B 88, 155119 (2013).Google Scholar
22. Cai, T., Li, X., Wang, F., Ju, S., Feng, J., and Gong, C.: Single-spin Dirac fermion and Chern insulator based on simple oxides. Nano Lett. 15, 6434 (2015).Google Scholar
23. Middey, S., Meyers, D., Kareev, M., Moon, E.J., Gray, B.A., Liu, X., Freeland, J.W., and Chakhalian, J.: Epitaxial growth of (111)-oriented LaAlO3/LaNiO3 ultra-thin superlattices. Appl. Phys. Lett. 101, 261602 (2012).Google Scholar
24. Liu, Xiaoran, Choudhury, D., Cao, Yanwei, Middey, S., Kareev, M., Meyers, D., Kim, J.-W., Ryan, P., and Chakhalian, J.: Epitaxial growth of (111)-oriented spinel CoCr2O4/Al2O3 heterostructures. Appl. Phys. Lett. 106, 071603 (2015).Google Scholar
25. Middey, S., Meyers, D., Doennig, D., Kareev, M., Liu, X., Cao, Y., Yang, Z., Shi, J., Gu, L., Ryan, P.J., Pentcheva, R., Freeland, J.W., and Chakhalian, J.: Mott electrons in an artificial graphenelike crystal of rare-earch nickelate. Phys. Rev. Lett. 116, 056801 (2016).Google Scholar
26. Hirai, D., Matsuno, J., and Takagi, H.: Fabrication of (111)-oriented Ca0.5Sr0.5IrO3/SrTiO3 superlattices—a designed playground for honeycomb physics. APL Mater. 3, 041508 (2015).CrossRefGoogle Scholar
27. Anderson, T.J., Ryu, S., Zhou, H., Xie, L., Podkaminer, J.P., Ma, Y., Irwin, J., Pan, X.Q., Rzchowski, M.S., and Eom, C.B.: Metastable honeycomb SrTiO3/SrIrO3 heterostructures. Appl. Phys. Lett. 108, 151604 (2016).Google Scholar
28. Panomsuwan, G., Takai, O., and Saito, N.: Epitaxial growth of (111)-oriented BaTiO3/SrTiO3 perovskite superlattices on Pt(111)/Ti/Al2O3 (0001) substrates. Appl. Phys. Lett. 103, 112902 (2013).Google Scholar
29. Mila, F.: Quantum spin liquids. Eur. J. Phys. 21, 499 (2000).Google Scholar
30. Bramwell, S.T. and Gingras, M.J.P.: Spin ice state in frustrated magnetic pyrochlore materials. Science 294, 1495 (2001).Google Scholar
31. Lee, S., Takagi, H., Louca, D., Matsuda, M., Ji, S., Ueda, H., Ueda, Y., Katsufuji, T., Chung, J., Park, S., Cheong, S., and Broholm, C.: Frustrated magnetism and cooperative phase transitions in spinels. J. Phys. Soc. Jpn. 79, 011004 (2010).CrossRefGoogle Scholar
32. Ramirez, A.P.: Strongly geometrically frustrated magnets. Annu. Rev. Mater. Sci. 24, 453 (1994).Google Scholar
33. Gardner, J.S., Gingras, M.J.P., and Greedan, J.E.: Magnetic pyrochlore oxides. Rev. Mod. Phys. 82, 53 (2010).Google Scholar
34. Binder, K. and Young, A.P.: Spin glass: experimental facts, theoretical concepts, and open questions. Rev. Mod. Phys. 58, 801 (1986).Google Scholar
35. Punk, M., Chowdhury, D., and Sachdev, S.: Topological excitations and the dynamic structure factor of spin liquids on the kagome lattice. Nat. Phys. 10, 289 (2014).Google Scholar
36. Pollmann, F., Fulde, P., and Shtengel, K.: Kinetic ferromagnetism on a kagome lattice. Phys. Rev. Lett. 100, 136404 (2008).CrossRefGoogle ScholarPubMed
37. Yu, S. and Li, J.: Chiral superconducting phase and chiral spin-density-wave phase in a Hubbard model on the kagome lattice. Phys. Rev. B 85, 144402 (2012).Google Scholar
38. Liu, Y., Kravstsov, V.C., Beauchamp, D.A., Eubank, J.F., and Eddaoudi, M.: 4-connected metal-organic assemblies mediated via heterochelation and bridging of single metal ions: kagome lattice and the M6L12 octahedron. J. Am. Chem. Soc. 127, 7266 (2005).Google Scholar
39. Nytko, E.A., Helton, J.S., Müller, P., and Nocera, D.G.: A structurally perfect S = ½ metal-organic hybrid kagome antiferromagnet. J. Am. Chem. Soc. 130, 2922 (2008).Google Scholar
40. Vaz, C.A.F., Henrich, V.E., Ann, C.H., and Altman, E.I.: Growth and characterization of thin epitaxial Co3O4 (111) films. J. Cryst. Growth 311, 2648 (2009).CrossRefGoogle Scholar
41. Liu, Xiaoran, Kareev, M., Cao, Y., Liu, J., Middey, S., Meyers, D., Freeland, J.W., and Chakhalian, J.: Electronic and magnetic properties of (111)-oriented CoCr2O4 epitaxial thin film. Appl. Phys. Lett. 105, 042401 (2014).Google Scholar
42. Yang, A., Chen, Z., Zuo, X., Kirkland, J., Vittoria, C., and Harris, V.G.: Cation-disorder-enhanced magnetization in pulsed-laser-deposition CuFe2O4 films. Appl. Phys. Lett. 86, 252510 (2005).Google Scholar
43. Ma, J.X., Mazumdar, D., Kim, G., Sato, H., Bao, N.Z., and Gupta, A.: A robust approach for the growth of epitaxial spinel ferrite films. J. Appl. Phys. 108, 063917 (2010).Google Scholar
44. Matzen, S., Moussy, J.-B., Mattana, R., Bouzehouane, K., Deranlot, C., Petroff, F., Cezar, J.C., Arrio, M.-A., Sainctavit, Ph., Gatel, C., Warot-Fonrose, B., and Zheng, Y.: Epitaxial growth and ferrimagnetic behavior of MnFe2O4 (111) ultrathin layers for room-temperature spin filtering. Phys. Rev. B 83, 184402 (2011).Google Scholar
45. Lüders, U., Bibes, M., Bobo, J., Cantoni, M., Bertacco, R., and Fontcuberta, J.: Enhanced magnetic moment and conductive behavior in NiFe2O4 spinel ultrathin films. Phys. Rev. B 71, 134419 (2005).Google Scholar
46. Chopdekar, R.V., Liberati, M., Takamura, Y., Kourkoutis, L.F., Bettinger, J.S., Nelson-Cheeseman, B.B., Arenholz, E., Doran, A., Scholl, A., Muller, D.A., and Suzuki, Y.: Magnetism at spinel thin film interfaces probed through soft X-ray spectroscopy techniques. J. Magn. Magn. Mater. 322, 2915 (2010).CrossRefGoogle Scholar
47. Yahiro, H., Tanaka, H., Yamamoto, Y., and Kawai, T.: Construction of ZnFe2O4/ZnGa2O4 spinel-type artificial superlattice by pulsed laser deposition. Jpn. J. Appl. Phys. 41, 5153 (2002).Google Scholar
48. Murata, T., Kozuka, Y., Uchida, M., and Kawasaki, M.: Magnetic properties of spin frustrated spinel ZnFe2O4/ZnCr2O4 superlattices. J. Appl. Phys. 118, 193901 (2015).Google Scholar
49. Wang, F. and Ran, Y.: Nearly flat band with Chern number C = 2 on the dice lattice. Phys. Rev. B 84, 241103(R) (2011).Google Scholar
50. Haldane, F.D.M.: Model for a quantum Hall effect without Landau levels: condensed matter realization of the “parity anomaly”. Phys. Rev. Lett. 61, 2015 (1988).Google Scholar
51. Rüegg, A., Mitra, C., Demkov, A.A., and Fiete, G.A.: Electronic structure of (LaNiO3)2/(LaAlO3) N heterostructures grown along [111]. Phys. Rev. B 85, 245131 (2012).Google Scholar
52. Rüegg, A., Mitra, C., Demkov, A.A., and Fiete, G.A.: Lattice distortion effects on topological phases in (LaNiO3)2/(LaAlO3) N heterostructures grown along the [111] direction. Phys. Rev. B 88, 115146 (2013).Google Scholar
53. Doennig, D., Pickett, W.E., and Pentcheva, R.: Confinement-driven transitions between topological and Mott phases in (LaNiO3) N /(LaAlO3) M (111) superlattices. Phys. Rev. B 89, 121110(R) (2014).Google Scholar
54. Weng, Y., Huang, X., Yao, Y., and Dong, S.: Topological magnetic phase in LaMnO3 (111) bilayer. Phys. Rev. B 92, 195114 (2015).Google Scholar
55. Tahini, H.A., Cossu, F., Singh, N., Smith, S.C., and Schwingenschlögl, U.: Electronic phase transitions under hydrostatic pressure in LaMnO3 (111) bilayers sandwiched between LaAlO3 . Phys. Rev. B 93, 035117 (2016).Google Scholar
56. Doennig, D., Baidya, S., Pickett, W.E., and Pentcheva, R.: Design of Chern and Mott insulators in buckled 3d oxide honeycomb lattices. Phys. Rev. B 93, 165145 (2016).Google Scholar
57. Ye, B., Mesaros, A., and Ran, Y.: Possible correlation-driven odd-parity superconductivity in LaNi7/8Co1/8O3 (111) bilayers. Phys. Rev. B 89, 201111(R) (2014).Google Scholar
58. Doennig, D., Pickett, W.E., and Pentcheva, R.: Massive symmetry breaking in LaAlO3/SrTiO3 (111) quantum wells: a three-orbital strongly correlated generalization of granphene. Phys. Rev. Lett. 111, 126804 (2013).CrossRefGoogle Scholar
59. Okamoto, S., Zhu, W., Nomura, Y., Arita, R., Xiao, D., and Nagaosa, N.: Correlation effects in (111) bilayers of perovskite transition-metal oxides. Phys. Rev. B 89, 195121 (2014).Google Scholar
60. Medarde, M.L.: Structural, magnetic and electronic properties of RNiO3 perovskites (R = rare earth). J. Phys. Condens. Matter 9, 1679 (1997).Google Scholar
61. Catalan, G.: Progress in perovskite nickelate research. Phase Transit. 81, 729 (2008).Google Scholar
62. Middey, S., Chakhalian, J., Mahadevan, P., Freeland, J.W., Millis, A.J., and Sarma, D.D.: Physics of ultrathin films and heterostructures of rare-earch nickelates. Annu. Rev. Mater. Res. 46, 305334 (2016).Google Scholar
63. Blok, J.L., Wan, X., Koster, G., Blank, D.H.A., and Rijnders, G.: Epitaxial oxide growth on polar (111) surfaces. Appl. Phys. Lett. 99, 151917 (2011).CrossRefGoogle Scholar
64. Middey, S., Rivero, P., Meyers, D., Kareev, M., Liu, X., Cao, Y., Freeland, J.W., Barraza-Lopez, S., and Chakhalian, J.: Polarity compensation in ultra-thin films of complex oxides: the case of a perovskite nickelate. Sci. Rep. 4, 6819 (2014).Google Scholar
65. Freeland, J.W., Tung, I.C., Luo, G., Zhou, H., Lee, J.H., Chang, S.H., Morgan, D., Bedzyk, M.J., and Fong, D.D.: Polarity and the metal-insulator transition in ultrathin LaNiO3 on SrTiO3, in APS March Meeting 2016, abstract #F30.00004 (2016).Google Scholar
66. Gibert, M., Zubko, P., Scherwitzl, R., Íñiguez, J., and Triscone, J.-M.: Exchange bias in LaNiO3–LaMnO3 superlattices. Nat. Mater. 11, 198 (2012).Google Scholar
67. Nogués, J., Sort, J., Langlais, V., Skumryev, V., Suriñach, S., Muñoz, J.S., and Baró, M.D.: Exchange bias in nanostructures. Phys. Rep. 422, 65 (2005).Google Scholar
68. Ali, M., Adie, P., Marrows, C.H., Greig, D., Hickey, B.J., and Stamps, R.L.: Exchange bias using a spin glass. Nat. Mater. 6, 60 (2007).Google Scholar
69. Dong, S. and Dagotto, E.: Quantum confinement induced magnetism in LaNiO3–LaMnO3 superlattices. Phys. Rev. B 87, 195116 (2013).Google Scholar
70. Lee, A.T. and Han, M.J.: Charge transfer, confinement, and ferromagnetism in LaMnO3/LaNiO3 (001) superlattices. Phys. Rev. B 88, 035126 (2013).Google Scholar
71. Piamonteze, C., Gibert, M., Heidler, J., Dreiser, J., Rusponi, S., Brune, H., Triscone, J.-M., Nolting, F., and Staub, U.: Interfacial properties of LaMnO3/LaNiO3 superlattices grown along (001) and (111) orientations. Phys. Rev. B 92, 014426 (2015).Google Scholar
72. Anderson, M.T., Greenwood, K.B., Taylor, G.A., and Poeppelmeier, K.R.: B-cation arrangements in double perovskites. Prog. Solid State Chem. 22, 197 (1993).CrossRefGoogle Scholar
73. Ramesh, R. and Spaldin, N.A.: Multiferroics: progress and prospects in thin films. Nat. Mater. 6, 21 (2007).Google Scholar
74. Singh, M.P., Truong, K.D., Jandl, S., and Fournier, P.: Multiferroic double perovskite: opportunities, issues, and challenges. J. Appl. Phys. 107, 09D917 (2010).Google Scholar
75. Shimakawa, Y., Azuma, M., and Ichikawa, N.: Multiferroic compounds with double-perovskite structures. Materials 4, 153 (2011).Google Scholar
76. Serrate, D., De Teresa, J.M., and Ibarra, M.R.: Double perovskites with ferromagnetism above room temperature. J. Phys.: Condens. Matter 19, 023201 (2007).Google Scholar
77. Zhang, H., Huang, H., Haule, K., and Vanderbilt, D.: Quantum anomalous Hall phase in (001) double-perovskite monolayers via intersite spin–orbit coupling. Phys. Rev. B 90, 165143 (2014).Google Scholar
78. Erten, O., Meetei, O., Mukherjee, A., Randeria, M., Trivedi, N., and Woodward, P.: Theory of half-metallic ferrimagnetism in double perovskites. Phys. Rev. Lett. 107, 257201 (2011).Google Scholar
79. Liu, Y., Fuh, H., and Wang, Y.: Ab Initio research on a new type of half-metallic double perovskite, A 2 Cr2MO6 (A = IVA group elements; M = Mo, Re and W). Computation 2, 12 (2014).Google Scholar
80. Ichikawa, N., Arai, M., Imai, Y., Hagiwara, K., Sakama, H., Azuma, M., Shimakawa, Y., Takano, M., Kotaka, Y., Yonetani, M., Fujisawa, H., Shimizu, M., Ishikawa, K., and Cho, Y.: Multiferrosim at room temperature in BiFeO3/BiCrO3 (111) artificial superlattices. Appl. Phys. Express 1, 101302 (2008).Google Scholar
81. Ueda, K., Tabata, H., and Kawai, T.: Ferromagnetism in LaFeO3–LaCrO3 superlattices. Science 280, 1064 (1998).Google Scholar
82. Ueda, K., Tabata, H., and Kawai, T.: Atomic arrangement and magnetic properties of LaFeO3–LaMnO3 artificial superlattices. Phys. Rev. B 60, R12561 (1999).Google Scholar
83. Chang, J., Lee, K., Jun, M., Kwon, J., Kim, M., and Kim, S.: Emergence of room-temperature magnetic ordering in artificially fabricated ordered-double-perovskite Sr2FeRuO6 . Chem. Mater. 23, 2693 (2011).Google Scholar
84. Kanamori, J.: Superexchange interaction and symmetry properties of electron orbitals. J. Phys. Chem. Solids 10, 87 (1959).Google Scholar
85. Pickett, W.E.: Ferromagnetic superlattices. Science 281, 1571a (1998).Google Scholar
86. Gray, B., Lee, H., Liu, J., Chakhalian, J., and Freeland, J.W.: Local electronic and magnetic studies of an artificial La2FeCrO6 double perovskite. Appl. Phys. Lett. 97, 013105 (2010).Google Scholar
87. Chakraveerty, S., Ohtomo, A., Okuyama, D., Saito, M., Okude, M., Kumai, R., Arima, T., Tokura, Y., Tsukimoto, S., Ikuhara, Y., and Kawasaki, M.: Ferrimagnetism and spontaneous ordering of transition metals in double perovskite La2CrFeO6 films. Phys. Rev. B 84, 064436 (2011).Google Scholar
88. Nechache, R., Carignan, L.-P., Gunawan, L., Harnagea, C., Botton, G.A., and Menard, D.: Epitaxial thin films of multiferroic Bi2FeCrO6 with B-site cationic order. J. Mater. Res. 22, 2102 (2007).Google Scholar
89. Yang, B. and Nagaosa, N.: Emergent topological phenomena in thin films of pyrochlore iridates. Phys. Rev. Lett. 112, 246402 (2014).Google Scholar
90. Fujita, T.C., Kozuka, Y., Uchida, M., Tsukazaki, A., Arima, T., and Kawasaki, M.: Odd-parity magnetoresistance in pyrochlore iridate thin films with broken time-reversal symmetry. Sci. Rep. 5, 9711 (2015).Google Scholar
91. Bovo, L., Moya, X., Prabhakaran, D., Soh, Y., Boothroyd, A.T., Mathur, N.D., Aeppli, G., and Bramwell, S.T.: Restoration of the third law in spin ice thin films. Nat. Commun. 5, 3439 (2014).Google Scholar
92. Fujita, T.C., Uchida, M., Kozuka, Y., Sano, W., Tsukazaki, A., Arima, T., and Kawasaki, M.: All-in-all-out magnetic domain wall conduction in a pyrochlore iridate heterointerface. Phys. Rev. B 93, 064419 (2016).Google Scholar
93. Chu, J., Riggs, S.C., Shapiro, M., Liu, J., Serero, C., Yi, D., Melissa, M., Suresha, S.J., Frontera, C., Vishwanath, A., Marti, X., Fisher, I.R., and Ramesh, R.: Linear magnetoresistance and time reversal symmetry breaking of pyrochlore iridates Bi2Ir2O7. arXiv:1309.4750.Google Scholar
94. Afonso, J.F. and Pardo, V.: Ab initio study of nontrivial topological phases in corundum-structured (M2O3)/(Al2O3)5 multilayers. Phys. Rev. B 92, 235102 (2015).Google Scholar
95. Ohtomo, A. and Hwang, H.Y.: A high-mobility electron gas at the LaAlO3/SrTiO3 heterointerface. Nature 427, 423 (2004).Google Scholar
96. Nakagawa, N., Hwang, H., and Muller, D.A.: Why some interfaces cannot be sharp. Nat. Mater. 5, 204 (2006).Google Scholar
97. Herranz, G., Sánchez, F., Dix, N., Scigaj, M., and Fontcuberta, J.: High mobility conduction at (110) and (111) LaAlO3/SrTiO3 interfaces. Sci. Rep. 2, 758 (2012).Google Scholar
98. Takei, S., Fregoso, B.M., Galitski, V., and Sarma, S.D.: Topological superconductivity and Majorana fermions in hybrid structures involving cuprate high-Tc superconductors. Phys. Rev. B 87, 014504 (2013).Google Scholar
99. Chakhalian, J., Freeland, J.W., Habermeier, H.-U., Cristiani, G., Khaliullin, G., van Veenendaal, M., and Keimer, B.: Orbital reconstruction and covalent bonding at an oxide interface. Science 318, 1114 (2007).Google Scholar
100. Catalano, S., Gibert, M., Bisogni, V., He, F., Sutarto, R., Viret, M., Zubko, P., Scherwitzl, R., Sawatzky, G.A., Schmitt, T., and Triscone, J.-M.: Tailoring the electronic transitions of NdNiO3 films through (111)pc oriented interfaces. APL Mater. 3, 062506 (2015).CrossRefGoogle Scholar
101. Ito, W., Mahajan, S., Yoshida, Y., Morishita, T., Kumagai, M., and Yabuta, K.: Influence of crystal strain on superconductivity of a-axis oriented YBa2Cu3Ox films. Jpn. J. Appl. Phys. 33, 5701 (1994).Google Scholar
102. Kim, T.H., Puggioni, D., Yuan, Y., Xie, L., Zhou, H., Campbell, N., Ryan, P.J., Choi, Y., Kim, J.-W., Patzner, J.R., Ryu, S., Podkaminer, J.P., Irwin, J., Ma, Y., Fennie, C.J., Rzchowski, M.S., Pan, X.Q., Gopalan, V., Rondinelli, J.M., and Eom, C.B.: Polar metals by geometric design. Nature 533, 68 (2016).Google Scholar
Figure 0

Figure 1. Schematic illustration of the idea about geometrical lattice engineering, which has three control parameters named as orientation, stacking, and superlattice throughout its entire process.

Figure 1

Figure 2. The conventional unit cell of a normal spinel structure. The corresponding (111) ionic planes are marked in the figures. Note, the A ionic planes only form the triangle planes, while the B ionic planes form both the triangle planes and also the kagome planes.

Figure 2

Figure 3. (111)-oriented CoCr2O4/Al2O3 (CCO/AlO) heterostructures. (a) Epitaxial relationship between CCO and AlO. The hexagonal close packing of AlO oxygen sublattice is labeled as AB in black, while the CCP of CCO oxygen sublattice is labeled as ABC in brown. (b)–(d) RHEED images during the growth of each component. The half-order reflections (marked by pink solid circles) observed on CCO layer is due to the double expansion of the in-plane unit cell. Reproduced from Ref. 24, with the permission of AIP Publishing.

Figure 3

Figure 4. (a) X-ray reflectivity and (b) x-ray diffraction curves of 2CCO/nAlO (n = 1 and 2) superlattices. Both the thickness fringes and the superlattice satellite peaks are clearly seen from the graphs. (c, d) x-ray absorption spectra of the CCO/AlO superlattices on the L2,3 edges of Co and Cr, respectively. The spectra of CCO powders with normal spinel structure are plotted as references [Figs4(a) and 4(b) adapted with permission of AIP Publishing from Ref. 46].

Figure 4

Figure 5. Buckled honeycomb lattice and Dice lattice geometry can be generated by epitaxial growth of perovskite system along the [111] direction. A sites are not shown for Dice lattice due to visual clarity.

Figure 5

Figure 6. (a) Schematics (assuming pure ionic picture) to demonstrate the presence (absence) of polar jump for RENiO3 on SrTiO3 (LaAlO3) (111) substrate[61]. (b) XAS of 5 uc LNO films on LAO and STO (111) have been compared with bulk Ni2+O, and LaNi3+O3. RHEED pattern of these films, recorded along pc [1−1 0]. For details, see Ref. 63. (c) Experimental arrangement for measuring XLD of (111)-oriented superlattice (upper panel) and XA spectra recorded for a [2NdNiO3/4LaAlO3]×3 SL grown on LAO (111) using vertically (V) and horizontally (H) polarized x-ray and their difference are plotted in lower panel. Due to strong overlap of Ni L3 edge with La M4 edge (from the substrate and spacer layer LAO), only Ni L2 edge is shown. Panel(c) adapted with permission from Ref. 25. Copyrighted by the American Physics Society.

Figure 6

Figure 7. B-site ordered double perovskites viewed along the conventional (001) and the unconventional (111) direction, respectively. The (001) rock-salt arrangement of the B and B′ sites is equivalent to (111) BO6 and B′O6 superlattice.

Figure 7

Figure 8. XAS and XMCD spectra on the L edge of (a) Fe and (b) Cr of the (111)-oriented 1LaFeO3/1LaCrO3 superlattice. Both spectra were measured at 10 K with an external magnetic field ~5 T applied parallel to the film surface. Data were collected in the total electron yield mode. Adapted from Ref. 86, with the permission of AIP Publishing.

Figure 8

Figure 9. Summary and outlook on GLE. The upper panel displays other possible routines to topological phase and frustrated magnetism by applying pure GLE. The bottom panel presents the combination of GLE with IE or SE to establish new systems with intriguing physics such as quasi-particle excitation and emergent phenomena.