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M A T E R I A L S S C I E N C E
Strain engineering of the magnetic multipole moments and anomalous Hall effect in pyrochlore iridate thin filmsWoo Jin Kim1,2*, Taekoo Oh1,2,3*, Jeongkeun Song1,2, Eun Kyo Ko1,2, Yangyang Li1,2, Junsik Mun4, Bongju Kim1,2, Jaeseok Son1,2, Zhuo Yang5, Yoshimitsu Kohama5, Miyoung Kim4, Bohm-Jung Yang1,2,3, Tae Won Noh1,2†
The recent observation of the anomalous Hall effect (AHE) without notable magnetization in antiferromagnets has suggested that ferromagnetic ordering is not a necessary condition. Thus, recent theoretical studies have proposed that higher-rank magnetic multipoles formed by clusters of spins (cluster multipoles) can generate the AHE without magnetization. Despite such an intriguing proposal, controlling the unconventional AHE by inducing these cluster multipoles has not been investigated. Here, we demonstrate that strain can manipulate the hidden Berry curvature effect by inducing the higher-rank cluster multipoles in spin-orbit–coupled antiferromagnets. Observing the large AHE on fully strained antiferromagnetic Nd2Ir2O7 thin films, we prove that strain-induced cluster T1-octupoles are the only source of observed AHE. Our results provide a previously unidentified pathway for generating the unconventional AHE via strain-induced magnetic structures and establish a platform for ex-ploring undiscovered topological phenomena via strain in correlated materials.
INTRODUCTIONThe anomalous Hall effect (AHE) is a fundamental transport phe-nomenon that has been universally observed in time-reversal sym-metry broken systems. AHE can arise from two different forms of mechanism (1): extrinsic mechanism, such as skew scattering or side jump due to magnetic impurities, and intrinsic mechanism originating from Berry curvature in momentum space. Since the fundamental topological properties of electronic wave functions are encoded in the Berry curvature, AHE is considered as a powerful tool for probing the topological properties of materials (2, 3). In addi-tion to its fundamental interest, AHE can be applied for memory devices (4).
Conventionally, AHE has been observed mostly in itinerant ferromagnets. Its magnitude is known to be proportional to the magnetization (5), which is a measure of broken time-reversal symmetry. Recently, a large AHE has been unexpectedly found in noncollinear antiferromagnets, such as Mn3X (X = Sn, Ge) (6–8) and GdPtBi (9), which do not exhibit spontaneous magnetization. This unconventional response indicates that ferromagnetism is not a necessary condition for AHE and suggests a possible alternative origin of AHE. A recent theory proposed that higher-rank magnetic multipole (cluster multipole) moments formed from spin clusters in antiferromagnet can induce a nonzero AHE, beyond the conventional dipoles of ferro-magnets (10). Subsequently, the anomalous Nernst (11) and magneto-optical Kerr effects (12) in Mn3Sn have also been attributed to its cluster octupoles. However, since antiferromagnets are not
easily coupled to both magnetic and electric fields (13), it is very difficult to manipulate the higher-rank cluster multipoles. This imposes substantial limitations on controlled experiments on the cluster multipoles and associated AHE.
Here, we demonstrate that the strain can generate the AHE by inducing the higher-rank cluster multipoles, by using antiferro-magnetic Nd2Ir2O7 (NIO) thin film. Further investigation reveals that biaxial strain on the pyrochlore lattice can modulate the spin structure and induce certain magnetic octupoles. The induced cluster octupoles can generate the net Berry curvature effect hidden in the bulk, leading to a finite AHE. We expect that our method could be widely applied to other spin-orbit–coupled topological magnets (10) and antiferromagnetic spintronics (4, 14).
RESULTSStrain-induced cluster multipoles in a pyrochlore latticeThe NIO belongs to the pyrochlore iridates family, R2Ir2O7 (R, rare- earth ions). The members of the family are geometrically frustrated magnets with complex lattice structures. As shown in Fig. 1A, R2Ir2O7 is composed of linked tetrahedrons with R and Ir at each vertex. In R2Ir2O7, strong electron correlations and large spin-orbit coupling of Ir d electrons result in unique antiferromagnetic spin structures, called all-in-all-out (AIAO) ordering (15, 16). As shown in the circle in Fig. 1B, the spins in one tetrahedron point inward and those in the neighboring tetrahedron point outward. The Néel temperatures of the Ir and Nd sublattices of bulk NIO are T N Ir ~ 30 K (15) and T N Nd ~ 15 K (17), respectively. This AIAO ordering breaks the time-reversal symmetry, allowing a nonzero Berry curvature distribution and generating correlated topological phases (18, 19) such as a Weyl semimetal.
However, since AIAO ordering preserves the cubic crystalline symmetry, the net Berry curvature effect vanishes when we integrate over the Brillouin zone (BZ). Unless the cubic crystalline symmetry is broken, AHE cannot be observed in this system. To break the
1Center for Correlated Electron Systems, Institute for Basic Science, Seoul 08826, Republic of Korea. 2Department of Physics and Astronomy, Seoul National University, Seoul 08826, Republic of Korea. 3Center for Theoretical Physics (CTP), Seoul National University, Seoul 08826, Republic of Korea. 4Department of Materials Science and Engineering and Research Institute of Advanced Materials, Seoul National University, Seoul 08826, Republic of Korea. 5Institute for Solid State Physics, The University of Tokyo, Kashiwa, Chiba 277-8581, Japan.*These authors contributed equally to this work.†Corresponding author. Email: [email protected]
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cubic symmetry, a magnetic field was applied to pressured NIO single crystals (19) and Pr-doped bulk samples (20, 21). However, the spin structures modulated by the magnetic field are fragile and easily re-turn once the magnetic field is turned off. Thus, a stable method to break the cubic symmetry is highly desirable; here, we choose a strain engineering approach and investigate the associated AHE.
As shown in Fig. 1B, the biaxial strain elongates the unit tetrahedra along the [111] direction. This will naturally break the cubic sym-metry of the system. Since the deformation modulates magnetic anisotropy (22), the Ir spin directions should be changed. To system-atically describe the change of spin direction, we adopted the cluster multipole theory. Since the conduction electrons come from Ir d orbitals, we considered Ir sublattice only (16). In the cubic pyrochlore lattice, all spin ordering patterns can be classified into five different irreducible representations, carrying 12 distinct cluster multipoles (18). Among them, certain cluster multipoles that break the cubic symmetry are responsible for the AHE (see section S1).
In a bulk NIO, the AIAO ordering corresponds to a higher-rank magnetic multipole called the A2-octupole (Fig. 1C). Since the A2-
octupole preserves the cubic symmetry, it cannot generate AHE. However, in a strained NIO (s-NIO), the AIAO spin structure becomes modulated under the strain. The resulting spin configuration is denoted by strained AIAO (s-AIAO), composed of a superposition of three kinds of cluster multipoles, namely, a dipole, an A2-octupole, and a T1-octupole (Fig. 1D). Note that the dipole is just the ferro-magnetic ordering, while the T1-octupole is an antiferromagnetic ordering other than AIAO. Only the T1-octupole can induce the AHE without magnetization since it breaks the cubic symmetry as the dipole does.
Characterizations of relaxed and fully s-NIO thin filmsTo investigate the strain-induced magnetic multipole and associated AHE, we prepared two kinds of NIO thin films on the yttria-stabilized zirconia (YSZ) substrates: relaxed and fully strained films. The biaxial strain can arise from the lattice mismatch between the R2Ir2O7 film and the YSZ substrate (see Fig. 1B) (23, 24). Since the lattice parameter of YSZ is smaller than those of NIO bulk, the NIO film should be compressively strained. We estimated the strain ( = 2 a YSZ − a NIO _ a NIO )
A
C
D
B
octupole
octupole
Fig. 1. The strain engineering concept used to induce magnetic multipoles in a pyrochlore lattice. (A) Pyrochlore lattice structure. Yellow (red) circles depict Nd (Ir) ions. Note that oxygen ions are not shown. (B) Schematic diagram of epitaxial NIO thin film on the yttria-stabilized zirconia (YSZ) substrate with biaxial strain along [111]. The deformed pyrochlore lattice is schematically displayed in the circle. The blue arrow at each site denotes the spin direction in the AIAO antiferromagnetic configuration. (C) The spin arrangement of a tetrahedron in the undistorted (i.e., bulk) AIAO configuration. According to the cluster magnetic multipole theory, the AIAO magnetic ordering can be represented as an A2-octupole. (D) Schematic diagram of the strained magnetic ground state. Biaxial strain along the [111] direction will distort the AIAO configuration, which can be represented as the superposition of a cluster dipole (M), an A2-octupole, and a T1-octupole (). M represents a ferromagnetic ordering, while represents an antiferromagnetic ordering other than AIAO. On the basis of symmetry analyses (see section S1 and table S1), we demonstrated that only the T1-octupole can induce the AHE without magnetization.
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to be −0.96%, where aNIO and aYSZ are lattice constants of bulk NIO (10.38 Å) and YSZ (5.14 Å), respectively.
Despite the substantial past efforts (25–27), the in situ growth of high-quality R2Ir2O7 thin film is notoriously difficult. Under the proper crystalline growth conditions for pyrochlore oxides (28), the corresponding R2Ir2O7 phase becomes extremely unstable because of the formation of a gaseous IrO3 phase (29). To avoid this instability, many studies have used the “solid-phase epitaxy (SPE)” (25, 27) method, which involves the initial growth of amorphous R2Ir2O7 films at a lower temperature (T) followed by ex situ thermal annealing in a sealed tube. Although SPE can provide a method for the growth of single-phase R2Ir2O7 films, it usually produces relaxed films (25, 26). Therefore, we developed a previously unknown in situ film growth method, i.e., repeated rapid high-temperature synthesis epitaxy (RRHSE; see section S2 and Materials and Methods) (30).
The RRHSE method made us successfully grow the fully s-NIO films on YSZ (111) substrates. Figure 2A shows an x-ray diffraction -2 scan. The NIO (lll) and YSZ (lll) (l: integer) peaks can be seen, indicating epitaxial growth of NIO single phase. Particularly, the satellite peaks near the NIO (222) peaks are observed, which is com-monly called “thickness fringes.” These interference peaks indicate the high quality of a sharp interface between film and substrate. Figure 2B shows x-ray reciprocal space mapping around the NIO (662) and YSZ (331) Bragg peaks of a 9-nm-thick NIO film. The lattice parameter of the (662)-plane, d(662), of bulk NIO is 1.19 Å, and the d(331) of YSZ is 1.18 Å. Note that the NIO (662) Bragg peak has the same Qx value as the YSZ (331) peak, demonstrating that our film becomes fully strained (~1% compressive strain) by the substrate.
Figure 2C shows a scanning transmission electron microscopy image that indicates the high quality of our film. The NIO pyrochlore phase is formed with few structural defects or disordered structures. Figure 2 (D and E) shows fast Fourier transform patterns from the selected areas in the film and substrate, respectively, marked in Fig. 2C. As demonstrated by the red dotted lines, the as-grown NIO film has the same inverse lattice constant as the YSZ substrate, which also confirms that our film is fully strained.
Electronic structures of relaxed and fully s-NIO thin filmsWe compared these fully s-NIO films grown by RRHSE with the relaxed NIO (r-NIO) films grown by the SPE (see section S3). The resistivity (T) curve of a 9-nm-thick s-NIO film exhibits a semi-metallic behavior at most T. As shown in Fig. 3A, the s-NIO film has (T) an order of magnitude smaller than that of the r-NIO film. The (T) curve of an 80-nm-thick r-NIO film exhibits a metal- insulator transition around ~30 K (black dashed line in Fig. 3A), in agreement with its bulk counterpart (17, 31). The strong upturn of the r-NIO film is due to its insulating nature below T N Ir ~ 30 K (17, 31). The (T) curve of the r-NIO film follows the Arrhenius plot (not shown here) in the low T region, indicating a bandgap opening. In contrast, the (T) curve of the s-NIO film has a positive slope for most T (orange line in Fig. 3A), suggesting that the film should be in a semimetallic state. Converting the resistivity into conductivity, the s-NIO film has xx ~ 1600 ohms−1 cm−1 at 2 K. The tiny upturn below ~30 K might arise from disorder effects.
To understand the corresponding electronic structure changes, we performed mean-field calculations using the Hubbard model (see section S4). The previous study shows that the most valence and conduction bands near the Fermi energy come mainly from Ir 5d electrons (16). Our calculated electronic structure of the bulk
(the r-NIO film in our case) explains its insulating nature. The energy gap opens with a value of about 13 meV (Fig. 3B), which agrees well with the bulk value (32). Under 1% compressive strain, the valence and conduction bands move, which slightly increases the direct gap at most k regions. However, some valence and conduction bands become crossed with Fermi level; thus, small electron and hole pockets develop near L1,2,3,4 (Fig. 3C), creating a semimetallic state. These model calculations can explain why the s-NIO film has a much smaller (T) than the r-NIO film.
Large AHE in fully s-NIO thin filmsBesides, the s-NIO film shows a much larger anomalous Hall conductivity (AHC) compared to the r-NIO film. Figure 3D shows the magnetic field (H)–dependent AHC xy A (H) at 2 K, obtained after subtracting the ordinary Hall contribution from the total Hall conductivity (see Materials and Methods). The xy A curves of s- and r-NIO films are displayed by the circles and the dashed line, respectively. The xy A (H = − 9 T) values of the s- and r-NIO films are 2.4 and 0.2 ohms−1 cm−1, respectively. The spontaneous Hall conductivity (SHC) xy A (H = 0) of the s-NIO films is 1.04 ohms−1 cm−1, which
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Z (2
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Z (1
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YSZ
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Fig. 2. Fully s-NIO thin film on a YSZ substrate, grown by the RRHSE method. (A) X-ray diffraction -2 scans of an epitaxial NIO film grown on a YSZ (111) substrate. The scans reveal that the NIO film was grown coherently with the YSZ substrate. (B) Reciprocal space mapping around the YSZ (331) and NIO (662) diffraction peaks. The Qx values of both peaks are the same, indicating that the film is under ~1% strain. (C) Scanning transmission electron microscopy image with the zone axis parallel to [1-10]; a clear interface between the film and the substrate can be seen. The distinctly colored circles indicate the pyrochlore structural ordering of the Nd and Ir ions. Images of selected areas in (C) were fast Fourier–transformed for (D) the NIO thin film, and (E) the YSZ substrate. The three vertical dotted lines between (D) and (E) are plotted without changing the scale. These lines indicate that the in-plane lattice constants of NIO and YSZ are the same, providing further direct evi-dence for the fully s-NIO thin film.
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is much larger than that of the r-NIO film. Note that the small AHC and SHC in the r-NIO film might be induced by the net mag-netization of AIAO domain walls (33). However, the large AHC and SHC in the s-NIO suggest that the net Berry curvature effect can be modulated by the strain.
To cross-check, we compared our magnetotransport property values with those of ferromagnets. For example, (Ga, Mn)As (34) and CuCr2Se4–xBrx (35) typically exhibit SHC with xy A (H = 0 T) ~ 1 to 10 ohms−1 cm−1 and xx(H = 0 T) ~ 1000 ohms−1 cm−1. These ferro-magnets follow a scaling relationship xy A ∝ xx 1.6 that implies the in-trinsic nature of the AHE (5). Since xy A and xx values for the s-NIO film also fall on the same scaling curve (see section S5), we con-firmed the enhanced AHC and SHC of our fully s-NIO film as the net Berry curvature effect.
Accordingly, we calculated the Berry curvature effect on AHC from the band structure obtained from the mean-field calculations mentioned above (see section S4). AHC can be obtained by integrat-ing the Berry curvature xy (
→ k ) throughout the whole BZ (5):
xy A = e 2 ℏ ∫ BZ
d 3 k (2) 3
∑ n f( ϵ n ( →
k ) − ) [111] ( →
k ) (1)
where f( ϵ n ( →
k ) − ) is the Fermi-Dirac distribution function and is the chemical potential. Figure 3E shows the Berry curvature [111] (
→ k ) of NIO along its high-symmetry lines with H = 0. Sizable [111]
( →
k ) at the L1,2,3,4 points in the BZ (Fig. 3F) exists for both the r- and s-NIO systems. The Berry curvature at each high-symmetry point for the r-NIO is somewhat larger than that for the 1% s-NIO. However, for the cubic r-NIO, xy A vanishes since the integration of Ω [111] (
→ k ) over
the BZ cancels out. Generally, when twofold rotation symmetries C2 about the x, y, or z axis exist, → Ω (
→ k ) is canceled by → Ω ( C 2
→ k ) . In the
r-NIO, all three C2 exist, so the net → Ω ( →
k ) contribution becomes hidden (9). In contrast, for the trigonal s-NIO, the breaking of all C2 sym-metries draw out a finite net → Ω (
→ k ) contribution. Thus, the biaxial
strain can promote the net Berry curvature effect originally hidden in the bulk, generating the large AHE in the s-NIO films.
Antihysteresis of AHCAnother notable feature of s-NIO film is that its xy A (H) curve shows an intriguing antihysteresis-like behavior, displayed in Fig. 3D. When we sweep the H-field from −9 to +9 T, a sign change occurs at an H value of about −1 T (circles in Fig. 3D). Similar behavior is also observed when we reverse the H-field sweep from +9 to −9 T. This H-dependent sign change of the AHC differs from a typical hysteretic response of most ferroic materials, where the sign change occurs during the domain switch to the opposite direction. Although a similar antihysteresis-like behavior has been also re-ported in an earlier Hall conductivity study of an NIO single crystal under hydrostatic high pressure (21), its origin has not fully in-vestigated yet.
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Γ Γ ΓL1 L2 L3 L4K2K1
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A ≠ 0
Fig. 3. Transport properties and electronic ground states of relaxed and fully s-NIO films. (A) Orange solid (black dashed) line indicates the resistivity, xx, of the fully s(r)-NIO film, prepared by the RRHSE (SPE) method. xx reveals that the electronic structure of NIO could be changed under strain. The calculated band structure of the (B) bulk and (C) 1% biaxial s-NIO is shown. The insulator-to-semimetal transition can explain the large change in xx in (A). (D) Measured AHC xy A of fully s-NIO (circle) and r-NIO (dashed line) films. Note that the xy A of s-NIO is an order of magnitude larger than that of r-NIO. Orange circles and dashed arrows depict H-field sweep results between −9 and 9 T; antihysteresis-like behavior can be seen. (E) Corresponding Berry curvature calculation results along the high-symmetry lines in (B) and (C). Although the Berry curvature of the bulk seems larger, the net contribution of xy ( → k ) becomes zero (i.e., hidden), resulting in xy A = 0 under cubic symmetry. On the other hand, the summation of the Berry curvature for the s-NIO could emerge because of the broken cubic symmetry. (F) Schematic of the BZ for the pyrochlore structure.
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To understand our antihysteresis-like xy A (H) curve, we used a phenomenological model (see section S6). The model is composed of two tangent hyperbolic functions; one is hysteretic (blue line) and the other is nonhysteretic (green line) (see Fig. 4A). Since the experimental data (orange circles) agree with the sum of two tangent hyperbolic functions (black solid line), the antihysteretic curve can be explained by the two different origins of xy A . To obtain further insight, we measured T-dependent xy A (H) curves of s-NIO film below 40 K. As shown in Fig. 4B, xy A does not exist at 40 K, when the system is in a paramagnetic phase. As T decreases, xy A starts to emerge at ~30 K and becomes stronger thereafter. In 15 K < T < 30 K, xy A ex-hibits no hysteretic behavior. However, as T decreases further below 15 K, xy A starts to show the antihysteresis-like behavior. Figure 4B shows that all T-dependent xy A curves are well matched with the sum of the nonhysteretic and hysteretic hyperbolic functions. Note that the bulk NIO has T N Nd ~ 15 K and T N Ir ~ 30 K (17), suggesting that the hysteretic and nonhysteretic responses are developed because of the magnetic orderings of Nd and Ir spins, respectively.
Figure 4C summarizes the results of the AHC fitting at H = −9 T with the T N Nd and T N Ir values, marked as the dotted lines. Note that, most transport in NIO occurs by Ir d electrons near the Fermi level. This carrier transport can be affected by the spin ordering at the Ir
and Nd sublattices. In Fig. 4C, the nonhysteretic component (green circles) starts to emerge below T N Ir , so it can be attributed to the Ir spin ordering, and we denote the nonhysteretic as xy Ir . On the other hand, the hysteretic component (blue circles) starts to emerge below T N Nd , so it can be attributed to the Nd spin ordering, and we denote the hysteretic as xy Nd . The nonhysteretic contribution of Ir is due to the absence of the Ir-AIAO domain switch by the smallness of Ir-AIAO coupling to the field. Meanwhile, the hysteretic contribution of Nd is due to the presence of the Ir-AIAO domain switch through f-d exchange with either Nd-3O1I or Nd-3I1O, which can be formed by large Nd moments under a [111] magnetic field (see section S6). This hysteretic behavior of xy Nd leads to the finite SHC at zero field xy A (H = 0 T) displayed as the red squares in Fig. 4C. Note that the SHC emerges below T N Nd .
AHE from strain-induced T1-octupolesTo reveal the relation of AHE and cluster multipoles under strain, we should compare M and xy A values (see Fig. 1D). The H-dependent M and xy A hysteresis curves at 3 K are displayed in Fig. 5A, and as-sociated xy Ir and xy Nd curves are shown in Fig. 5B. Figure 5A demonstrates that the conventional understanding of the SHC (5), i.e., xy A (H = 0 T ) ∝ M (0 T), does not hold for the s-NIO film. Although the s-NIO film has a large SHC signal (orange circles) shown in Fig. 5A, it has no spontaneous M at 3 K with H = 0 (purple squares) within the measurement error (± 0.01 B/NdIrO3.5). As shown in Fig. 1D, the biaxial deformation of pyrochlore lattice can generate three kinds of multipoles, i.e., a dipole, an A2-octupole, and a T1- octupole. The dipole is crossed out because of the zero magnetization of our data, and the A2-octupole is crossed out because of its zero con-tribution to AHC. Therefore, the strain-induced T1-octupole should play important roles in generating the AHC without magnetization.
To elucidate how T1-octupole emerges under the strain, we cal-culated the spin structure from the spin model. Since both Nd and Ir spins play important roles, we included the Heisenberg, Dzyaloshinskii-Moriya, anisotropic spin-exchange interactions be-tween Ir spins (36), the f-d exchange interaction between the Ir and Nd spins (17), and the Zeeman energy for both the Ir and Nd spins (for details, see section S7). On the basis of the calculated spin structure, we obtained the cluster multipoles (table S1 in section S1). Figure 5C shows the calculated dipole (M, green circles) and T1-octupole (, blue circles) as a function of the effective Zeeman energy h in the r-NIO. According to our calculation, r-NIO does not have a finite M or value for the Ir sublattice at h = 0. The zero values of M and can explain the negligible SHC of the r-NIO film (see Fig. 3D). Figure 5D shows the calculated M and of s-NIO, which are finite even for h = 0. Particularly, the hysteresis curve of looks similar to the xy Nd curve in Fig. 5B. Therefore, we conclude that the large spon-taneous that generate AHE can be induced by the strain in the s-NIO film.
DISCUSSIONOur work demonstrates that the strain-engineering of an antiferro-magnet can generate the net Berry curvature effects by modulating its cluster multipoles. In particular, our findings highlight that the strain-induced T1-octupole is closely connected with the topological properties of NIO. We can further extend this strain-engineering approach to search for the other novel topological phenomena in correlated magnets. For example, the strain engineering approach
A B
C
Fig. 4. T-dependent AHC and occurrence of SHC below T N Nd . (A) AHC xy A at T = 3 K. The orange circles are the measured values. The blue (green) line indicates a fitting curve for the Nd (Ir) spin contribution, i.e., xy Nd ( xy Ir ), obtained from the pheno-menological model (see main text). The black line is the sum of xy Nd and xy Ir . AOAI, all-out-all-in. (B) T-dependent xy A . The orange circles (black solid lines) depict the experimental results (fitting curves). Near T ~ T N Ir (~ 30 K), AHC starts to emerge, which indicates the Ir spin ordering effect. Below T ~ T N Nd (~ 15 K), AHC starts to ex-hibit hysteretic behavior, indicating that Nd spin ordering plays an important role via the f-d exchange interaction. (C) T-dependent contributions of Ir and Nd spins to AHC, i.e., xy Ir (H = − 9 T) (green circles) and xy Nd (H = −9 T) (blue circles). The red squares indicate the SHC values, i.e., AHC without magnetic field | xy A (H = 0 T)|. Note that SHC develops below T N Nd ~ 15 K.
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on numerous series of R2Ir2O7 can realize novel correlated topological phases, such as Weyl semimetal, axion insulator (16), a strong topo-logical insulator (18), and line-node semimetal (19, 21) by properly modifying their magnetic structure. In this perspective, we believe that our strain study on NIO could provide a cornerstone to discov-er strain-engineered novel topological phenomena in oxides and to understand their fundamental mechanisms.
MATERIALS AND METHODSFilm growth and structural characterizationFully s-NIO films were in situ grown on insulating YSZ substrates using the RRHSE method. This film growth method is a modi-fied form of pulsed laser deposition, based on repeated short-term thermal annealing processes using an infrared laser. RRHSE con-sists of two key steps in one thermal cycle. During the first step, amorphous stoichiometric NIO and IrO2 layers were deposited by a KrF excimer laser ( = 248 nm, 5 Hz) at T ~ 600°C with PO2 ~ 50 mtorr. The additional IrO2 layer was deposited to compensate for the Ir loss that would unavoidably occur later during the synthesis process. During the second step, the pyrochlore phase is formed by rapidly raising T to 800°C (up to ~400°C min−1). We must expose the sample to the high T for a period that is sufficiently long to syn-thesize the pyrochlore phase but short enough to minimize the formation of IrO3. Last, we repeated these deposition and thermal synthesis processes until the desired film thickness was obtained. During the growth, the reflection high-energy electron diffraction
pattern was monitored and the intensity of the oscillation was re-corded. After growth, NIO films were characterized by an x-ray dif-fractometer (Bruker Corp.) and an atomic-resolution high-angle annular dark-field scanning transmission electron microscope (JEM-ARM200F; JEOL) equipped with an energy-dispersive x-ray spectrometer.
Transport and magnetic propertiesMagnetotransport properties were measured via a standard four- point probe method using a commercial physical property measure-ment system (PPMS, Quantum Design), which has a base T of 2 K and a maximum magnetic field of 9 T. During the measurements, the current was applied along the [1-10] direction, and H was applied along the [111] direction. Magnetization data were obtained using a commercial superconducting quantum interference device magnetometer (MPMS, Quantum Design) with the magnetic field applied normal to the film.
The AHC value xy A can be obtained from the resistivity values,
namely, xy A (H ) = xy A (H) ___________ xx (H) 2 + xy A (H) 2
where xy A is anomalous Hall resist-
ivity and xx is longitudinal resistivity. To exclude the longitudinal contribution from the raw Hall resistivity data xy r , we used the antisymmetrization procedure (8, 9, 13). We separated the positive and negative field sweep branches and then antisymmetrized xy using xy + (H) = xy r+ (H ) − xy r− (− H) _ 2 and xy − (H) = xy r− (H ) − xy r+ (− H) _ 2 . Note that xy r+ (H) and xy r− (H) denote positive field sweep (+9 T to −9 T) and negative field sweep (−9 T to +9 T) branches, respectively. From xy + (H) and xy − (H) , we took out the linear part (ordinary Hall resistivity) to determine xy A .
Self-consistent mean-field Hubbard modelWe developed the Hubbard model for the s-NIO thin film under the magnetic field and acquired the ground state and electronic structure by the self-consistent mean-field method. We adopted 24 × 24 × 24 and 32 × 32 × 32 k-point mesh and found that the re-sults are consistent. We calculated the AHC by integrating the Berry curvature, adopting a 48 × 48 × 48 k-point mesh of the entire BZ. Details of the calculation are provided in section S4.
Spin model calculationWe developed the spin model including Heisenberg exchange, Dzyaloshinskii-Moriya interaction, anisotropic exchange, the f-d exchange between Nd and Ir electrons, and the Zeeman effect by applying second-order perturbation theory to the Hubbard model and referring to previous works. We calculated the ground state by the iterative minimization method, which repeatedly aligns spins to the effective field direction until each spin is fixed. Details of the calculation are provided in section S7.
SUPPLEMENTARY MATERIALSSupplementary material for this article is available at http://advances.sciencemag.org/cgi/content/full/6/29/eabb1539/DC1
REFERENCES AND NOTES 1. N. Nagaosa, J. Sinova, S. Onoda, A. H. MacDonald, N. P. Ong, Anomalous Hall effect.
Rev. Mod. Phys. 82, 1539–1592 (2010). 2. A. A. Burkov, Anomalous Hall effect in Weyl metals. Phys. Rev. Lett. 113, 187202 (2014). 3. S. Nishihaya, M. Uchida, Y. Nakazawa, R. Kurihara, K. Akiba, M. Kriener, A. Miyake,
Y. Taguchi, M. Tokunaga, M. Kawasaki, Quantized surface transport in topological Dirac semimetal films. Nat. Commun. 10, 2564 (2019).
A
C
B
D
Fig. 5. Emergence of strain-induced magnetic multipoles and their relation to AHC in NIO. (A) The M/H curve (purple squares) of s-NIO film at 3 K, overlaid with the experimental AHC (orange circles). Note that M = 0 but xy A ≠ 0 without H. The nonzero value of xy A at H = 0 and M = 0 indicates an alternative origin of the AHE. (B) The AHC of s-NIO film at 3 K. The orange circles are experimental data. The green line is the contribution of Ir spins, i.e., xy Ir , based on our model calculation (see Fig. 4A). The blue solid and dashed lines are the contributions of Nd spins, i.e., xy Nd , during decreasing and increasing h-sweeps, respectively. Calculated magnetic multipoles in NIO under the effective Zeeman energy, h, (C) without and (D) with 1% strain are shown. The green and blue circles indicate dipole M and T1-octupole , respectively. The strain-induced becomes the origin of the SHC in our s-NIO film.
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7 of 7
4. L. Šmejkal, Y. Mokrousov, B. Yan, A. H. MacDonald, Topological antiferromagnetic spintronics. Nat. Phys. 14, 242–251 (2018).
5. M. Onoda, N. Nagaosa, Topological nature of anomalous Hall effect in ferromagnets. J. Physical Soc. Japan 71, 19–22 (2002).
6. S. Nakatsuji, N. Kiyohara, T. Higo, Large anomalous Hall effect in a non-colinear antiferromagnet at room temperature. Nature 527, 212–215 (2015).
7. N. Kiyohara, T. Tomita, S. Nakatsuji, Giant anomalous Hall effect in the chiral antiferromagnet Mn3 Ge. Phys. Rev. Appl. 5, 064009 (2016).
8. A. K. Nayak, J. E. Fischer, Y. Sun, B. Yan, J. Karel, A. C. Komarek, C. Shekhar, N. Kumar, W. Schnelle, J. Kübler, C. Felser, S. S. P. Parkin, Large anomalous Hall effect driven by a nonvanishing Berry curvature in the noncolinear antiferromagnet Mn3Ge. Sci. Adv. 2, e1501870 (2016).
9. T. Suzuki, R. Chisnell, A. Devarakonda, Y.-T. Liu, W. Feng, D. Xiao, J. W. Lynn, J. G. Checkelsky, Large anomalous Hall effect in a half-Heusler antiferromagnet. Nat. Phys. 12, 1119–1123 (2016).
10. M.-T. Suzuki, T. Koretsune, M. Ochi, R. Arita, Cluster multipole theory for anomalous Hall effect in antiferromagnets. Phys. Rev. B 95, 094406 (2017).
11. M. Ikhlas, T. Tomita, T. Koretsune, M.-T. Suzuki, D. N. Hamane, R. Arita, Y. Otani, S. Nakatsuji, Large anomalous Nernst effect at room temperature in a chiral antiferromagnet. Nat. Phys. 13, 1085–1090 (2017).
12. T. Higo, H. Man, D. B. Gopman, L. Wu, T. Koretsune, O. M. J. van’t Erve, Y. P. Kabanov, D. Rees, Y. Li, M.-T. Suzuki, S. Patankar, M. Ikhlas, C. L. Chien, R. Arita, R. D. Shull, J. Orenstein, S. Nakatsuji, Large magneto-optical Kerr effect and imaging of magnetic octupole domains in an antiferromagnetic metal. Nat. Photonics 12, 73–78 (2018).
13. T. Ohuchi, J. Matsuno, N. Ogawa, Y. Kozuka, M. Uchida, Y. Tokura, M. Kawasaki, Electric-field control of anomalous and topological Hall effects in oxide bilayer thin films. Nat. Commun. 9, 213 (2018).
14. T. Jungwirth, X. Marti, P. Wadley, J. Wunderlich, Antiferromagnetic spintronics. Nat. Nanotechnol. 11, 231–241 (2016).
15. K. Matsuhira, M. Wakeshima, Y. Hinatsu, S. Takagi, Metal–insulator transitions in pyrochlore oxides Ln2Ir2O7. J. Physical Soc. Japan 80, 094701 (2011).
16. X. Wan, A. M. Turner, A. Vishwanath, S. Y. Savrasov, Topological semimetal and Fermi-arc surface states in the electronic structure of pyrochlore iridates. Phys. Rev. B 83, 205101 (2011).
17. Z. Tian, Y. Kohama, T. Tomita, H. Ishizuka, T. H. Hsieh, J. J. Ishikawa, K. Kindo, L. Balents, S. Nakatsuji, Field-induced quantum metal–insulator transition in the pyrochlore iridate Nd2Ir2O7. Nat. Phys. 12, 134 (2016).
18. B.-J. Yang, Y. B. Kim, Topological insulators and metal-insulator transition in the pyrochlore iridates. Phys. Rev. B 82, 085111 (2010).
19. T. Oh, H. Ishizuka, B.-J. Yang, Magnetic field induced topological semimetals near the quantum critical point of pyrochlore iridates. Phys. Rev. B 98, 144409 (2018).
20. K. Ueda, T. Oh, B.-J. Yang, R. Kaneko, J. Fujioka, N. Nagaosa, Y. Tokura, Magnetic-field induced multiple topological phases in pyrochlore iridates with Mott criticality. Nat. Commun. 8, 15515 (2017).
21. K. Ueda, R. Kaneko, H. Ishizuka, J. Fujioka, N. Nagaosa, Y. Tokura, Spontaneous Hall effect in the Weyl semimetal candidate of all-in all-out pyrochlore iridate. Nat. Commun. 9, 3032 (2018).
22. B.-J. Yang, N. Nagaosa, Emergent topological phenomena in thin films of pyrochlore iridates. Phys. Rev. Lett. 112, 246402 (2014).
23. X. Ke, T. Birol, R. Misra, J.-H. Lee, B. J. Kirby, D. G. Schlom, C. J. Fennie, J. W. Freeland, Structural control of magnetic anisotropy in a strain-driven multiferroic EuTiO3 thin film. Phys. Rev. B 88, 094434 (2013).
24. K.-Y. Yang, Y.-M. Lu, Y. Ran, Quantum Hall effects in a Weyl semimetal: Possible application in pyrochlore iridates. Phys. Rev. B 84, 075129 (2011).
25. J. C. Gallagher, B. D. Esser, R. Morrow, S. R. Dunsiger, R. E. A. Williams, P. M. Woodward, D. W. McComb, F. Y. Yang, Epitaxial growth of iridate pyrochlore Nd2Ir2O7 films. Sci. Rep. 6, 22282 (2016).
26. W. C. Yang, Y. T. Xie, W. K. Zhu, K. Park, A. P. Chen, Y. Losovyj, Z. Li, H. M. Liu, M. Starr, J. A. Acosta, C. G. Tao, N. Li, Q. X. Jia, J. J. Heremans, S. X. Zhang, Epitaxial thin films of pyrochlore iridate Bi2+xIr2-yO7-: Structure, defects and transport properties. Sci. Rep. 7, 7740 (2017).
27. T. C. Fujita, Y. Kozuka, M. Uchida, A. Tsukazaki, T. Arima, M. Kawasaki, Odd-parity magnetoresistance in pyrochlore iridate thin films with broken time-reversal symmetry. Sci. Rep. 5, 9711 (2015).
28. K. T. Jacob, T. H. Okabe, T. Uda, Y. Waseda, Solid-state cells with buffer electrodes for accurate thermodynamic measurements: System Nd-Ir-O. Electrochim. Acta 45, 1963–1971 (2000).
29. C. B. Alcock, G. W. Hooper, Thermodynamics of the gaseous oxides of the platinum-group metals. Proc. R. Soc. London. Ser. A. Math. Phys. Sci. 254, 551–561 (1960).
30. W. J. Kim, E. K. Kyo, S. Y. Kim, B. Kim, T. W. Noh, In-operando spectroscopic ellipsometry studies of IrO2 dynamic instabilities: Guide to in-situ growth of pyrochlore iridate thin films. Curr. Appl. Phys. 19, 400–405 (2019).
31. K. Ueda, J. Fujioka, B.-J. Yang, J. Shiogai, A. Tsukazaki, S. Nakamura, S. Awaji, N. Nagaosa, Y. Tokura, Magnetic field-induced insulator-semimetal transition in a pyrochlore Nd2Ir2O7. Phys. Rev. Lett. 115, 056402 (2015).
32. M. Nakayama, T. Kondo, Z. Tian, J. J. Ishikawa, M. Halim, C. Bareille, W. Malaeb, K. Kuroda, T. Tomita, S. Ideta, K. Tanaka, M. Matsunami, S. Kimura, N. Inami, K. Ono, H. Kumigashira, L. Balents, S. Nakatsuji, S. Shin, Slater to Mott crossover in the metal to insulator transition of Nd2Ir2O7. Phys. Rev. Lett. 117, 056403 (2016).
33. W. J. Kim, J. H. Gruenewald, T. Oh, S. Cheon, B. Kim, O. B. Korneta, H. Cho, D. Lee, Y. Kim, M. Kim, J.-G. Park, B.-J. Yang, A. Seo, T. W. Noh, Unconventional anomalous Hall effect from antiferromagnetic domain walls of Nd2Ir2O7 thin films. Phys. Rev. B 98, 125103 (2018).
34. D. Chiba, Y. Nishitani, F. Matsukura, H. Ohno, Properties of Ga1−x Mnx As with high Mn composition (x > 0.1). Appl. Phys. Lett. 90, 122503 (2007).
35. W.-L. Lee, S. Watauchi, V. L. Miller, R. J. Cava, N. P. Ong, Dissipationless anomalous Hall current in the ferromagnetic spinel CuCr2Se4-xBrx. Science 303, 1647–1649 (2004).
36. G. Sim, S. Lee, Discovery of a new type of magnetic order on pyrochlore spinels. Phys. Rev. B 98, 014423 (2018).
37. W. Witczak-Krempa, A. Go, Y. B. Kim, Pyrochlore electrons under pressure, heat, and field: Shedding light on the iridates. Phys. Rev. B 87, 155101 (2013).
38. W. Harrison, Electronic Structure and the Properties of Solids: The Physics of the Chemical Bond (Dover Publications, 1989).
39. K. Ohgushi, S. Murakami, N. Nagaosa, Spin anisotropy and quantum Hall effect in the kagomé lattice: Chiral spin state based on a ferromagnet. Phys. Rev. B 62, R6065–R6068 (2000).
40. E. Y. Ma, Y.-T. Cui, K. Ueda, S. Tang, K. Chen, N. Tamura, P. M. Wu, J. Fujioka, Y. Tokura, Z.-X. Shen, Mobile metallic domain walls in an all-in-all-out magnetic insulator. Science 350, 538 (2015).
Acknowledgments: We acknowledge the invaluable comments and suggestions from D. Lee, S. H. Chang, T. H. Kim, and C. H. Sohn. Funding: This work was supported by the Research Center Program of the Institute for Basic Science in Korea (grants no. IBS-R009-D1 and no. IBS-R009-G1). T.O. and B.-J.Y. acknowledge the support by the Institute for Basic Science in Korea (Grant No. IBS-R009-D1), Basic Science Research Program through the National Research Foundation of Korea (NRF) (Grant No. 0426-20200003), and the U.S. Army Research Office under Grant Number W911NF-18-1-0137. STEM measurement was supported by the National Center for Inter-University Research Facilities (NCIRF) at Seoul National University in Korea. Author contributions: W.J.K., T.O., B.-J.Y., and T.W.N. conceived the original idea. W.J.K. and T.W.N designed the experiments. T.O. performed the tight-binding model calculations and spin model calculations under the supervision of B.-J.Y. J.M. performed the STEM measurements under the supervision of M.K., W.J.K., J.Song, and E.K.K. grew and characterized the structure of the samples. W.J.K., J.Song, Y.L., Z.Y., and Y.K. performed the magnetotransport measurements. W.J.K., T.O., J.Song, B.-J.Y., and T.W.N. analyzed the results and wrote the manuscript with contribution from all authors. All authors participated in the discussion during the manuscript preparation. Competing interests: The authors declare that they have no competing interests. Data and materials availability: All data needed to evaluate the conclusions in the paper are present in the paper and/or the Supplementary Materials. Additional data related to this paper may be requested from the authors.
Submitted 4 February 2020Accepted 29 May 2020Published 15 July 202010.1126/sciadv.abb1539
Citation: W. J. Kim, T. Oh, J. Song, E. K. Ko, Y. Li, J. Mun, B. Kim, J. Son, Z. Yang, Y. Kohama, M. Kim, B.-J. Yang, T. W. Noh, Strain engineering of the magnetic multipole moments and anomalous Hall effect in pyrochlore iridate thin films. Sci. Adv. 6, eabb1539 (2020).
pyrochlore iridate thin filmsStrain engineering of the magnetic multipole moments and anomalous Hall effect in
Yoshimitsu Kohama, Miyoung Kim, Bohm-Jung Yang and Tae Won NohWoo Jin Kim, Taekoo Oh, Jeongkeun Song, Eun Kyo Ko, Yangyang Li, Junsik Mun, Bongju Kim, Jaeseok Son, Zhuo Yang,
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