With large spin-orbit coupling, the electron configuration in d-metal oxides is prone to highly anisotropic exchange interactions and exotic magnetic properties. In 5d5 iridates, given the existing variety of crystal structures, the magnetic anisotropy can be tuned from antisymmetric to symmetric Kitaev-type, with interaction strengths that outsize the isotropic terms. By many-body electronic-structure calculations we here address the nature of the magnetic exchange and the intriguing spin-glass behavior of Li2RhO3, a 4d5 honeycomb oxide. For pristine crystals without Rh-Li site inversion, we predict a dimerized ground state as in the isostructural 5d5 iridate Li2IrO3, with triplet spin dimers effectively placed on a frustrated triangular lattice. With Rh-Li anti-site disorder, we explain the observed spin-glass phase as a superposition of different, nearly degenerate symmetry-broken configurations.
For d-metal compounds with localized magnetic moments, basic guidelines to soothsay the sign of the nearest-neighbor (NN) magnetic exchange interactions, i. e., the Anderson-Goodenough-Kanamori rules1,2,3, were laid down back in the 1950’s. With one single bridging anion and half-filled d states these rules safely predict antiferromagnetic (AF) exchange interactions, as is indeed encountered in numerous magnetic Mott insulators. It is however much harder to anticipate the sign of the couplings for geometries with two bridging ligands and bond angles close to 90°. Illustrative recent examples are the 5d honeycomb systems Na2IrO3 and Li2IrO3. The signs of the NN Heisenberg J and of the additional symmetric Kitaev anisotropy K are intensely debated in these iridates, with both J < 0, K > 04,5,6 and J > 0, K < 07,8,9,10,11,12 sets of parameters being used to explain the available experimental data.
The sizable Kitaev interactions, that is, uniaxial symmetric terms that cyclically permute on the bonds of a particular hexagonal ring13,14,15, are associated to strong frustration effects and unconventional magnetic ground states displaying, for example, noncollinear order, incommensurability, or spin-liquid behavior4,5,6,7,8,11,12,15,16,17. Obviously, in the context of electronic-structure computational methods, such features cannot be thoroughly addressed by periodic total-energy calculations for a given set of predetermined spin configurations. A much more effective strategy is to first focus on individual pairs of NN d-metal sites and obtain reliable values for the associated effective magnetic couplings by using ab initio many-body quantum chemistry (QC) machinery (for a recent review, see ref. 18). The computed exchange parameters can be subsequently fed to effective spin Hamiltonians to be solved for larger sets of magnetically active lattice sites. Such an approach, earlier, allowed us to establish the signs plus the relative strengths of the Heisenberg and Kitaev interactions in both Na2IrO3 and Li2IrO3 and to additionally rationalize the qualitatively different types of AF orders in these two 5d5 honeycomb iridates16,17.
The related 4d5 honeycomb compound Li2RhO3 is even more puzzling because it features no sign of long-range magnetic order. Instead, an experimental study suggests the presence of a spin-glass ground state19. While the spin-orbit couplings (SOC’s) are still sizable for the 4d shell and may in principle give rise on the honeycomb lattice to compelling Kitaev physics, to date no conclusive evidence is in this respect available for Li2RhO3. To shed light on the nature of the essential exchange interactions in Li2RhO3 we here carry out detailed ab initio QC calculations. We show that large trigonal splittings within the Rh t2g shell, comparable with the strength of the SOC, dismiss a simple picture based on jeff = 1/2 and jeff = 3/2 effective states14,20,21,22. The magnetic properties of the system can still be described, however, in terms of pseudospins. The calculations earmark Li2RhO3 as a 4d-electron system with remarkably large anisotropic magnetic couplings, in particular, FM Kitaev interactions of up to 10–15 meV. The isotropic Heisenberg exchange, on the other hand, features opposite signs on the two sets of structurally distinct links of Rh NN’s. This sign modulation of the NN Heisenberg interactions, with strong ferromagnetic (FM) J’s for one type of Rh-Rh bonds and weaker AF couplings for the other pairs of adjacent Rh sites, enables the initial hexagonal network to be mapped onto an effective model of spin-1 dimers on a frustrated triangular lattice. We further address the issue of Rh-Li anti-site disorder in samples of Li2RhO3. By exact-diagonalization (ED) calculations for an extended spin model that also includes second and third neighbor couplings, we show that the experimentally observed spin-glass behavior can be rationalized as a superposition of different nearly-degenerate symmetry-broken states arising at finite concentration of in-plane spin vacancies.
Rh4+ 4d5 electronic structure
The tetravalent rhodium ions in Li2RhO3 display a 4d5 valence electron configuration, octahedral ligand coordination and bonding through two bridging ligands. In the simplest picture, i.e., for sufficiently large Rh t2g − eg splittings and degenerate t2g levels, the ground-state electron configuration at each site is a effective jeff = 1/2 spin-orbit doublet14,20,21,22. For 5d5 ions in a variety of three-dimensional, layered and chain-like oxides, ab initio QC electronic-structure calculations yield excitation energies of 0.6–0.9 eV for the transitions between the j ≈ 1/2 and split j ≈ 3/2 levels23,24,25,26 and indicate values of 0.45–0.5 eV for the strength of the SOC λ, in agreement with earlier estimates27. Sharp features in the range of 0.6–0.9 eV are indeed found in the resonant x-ray scattering spectra23,24,25,28.
The validity of the jeff = 1/2 approximation for the ground state of Li2RhO3 is however questionable since the SOC is substantially weaker for 4d elements. Indeed our QC calculations (see Table 1) indicate Rh t2g splittings δ ≈ 0.11 eV, close to values of 0.14–0.16 eV estimated for λ in various Rh4+ oxides26,29. For the ab initio QC investigation we employed multiconfiguration complete-active-space self-consistent-field (CASSCF) and multireference configuration-interaction (MRCI) calculations30, see Supplemental Material (SM) and refs 23,26. With δ and λ parameters of similar size, the jeff = 1/2 and jeff = 3/2 states are strongly admixed, as discussed in earlier work20,31 and illustrated in Table 1. In particular, for the relativistic ground-state wave function the t2g hole is not equally distributed among the three Rh t2g levels as for the “true” jeff = 1/2 ground state20,21 but displays predominant dxy character, close to 60%.
Magnetic couplings between two adjacent Rh4+ ions
Interestingly, while the results for the on-site 4d5 excitations are quite different as compared to the 5d5 excitation energies23, the computed intersite effective interactions are qualitatively similar to those obtained for the 5d5 honeycomb iridate Li2IrO317. The intersite exchange couplings were estimated by MRCI + SOC calculations for embedded fragments having two edge-sharing IrO6 octahedra in the active region. As described in earlier work16,17,32 and in SM, the ab initio QC data for the lowest four spin-orbit states describing the magnetic spectrum of two NN octahedra is mapped in our scheme onto an effective spin Hamiltonian including both isotropic Heisenberg exchange and symmetric anisotropy. Yet the spin-orbit calculations, CASSCF or MRCI, incorporate all nine triplet and nine singlet states that arise from the two-site configuration.
For on-site Kramers-doublet configurations, the most general symmetry-allowed form of the effective spin Hamiltonian, for a pair of NN ions, is
where , are 1/2 pseudospin operators, J is the isotropic Heisenberg interaction, K the Kitaev coupling and the coefficients are off-diagonal elements of the symmetric anisotropic exchange matrix with . The antisymmetric anisotropic term vanishes since the crystallographic data reported in ref. 33 indicate overall C2 h point-group symmetry for one block of NN RhO6 octahedra, green (B1) bonds in Fig. 1 and only slight deviations from C2 h for the other type of NN’s, blue (B2 and B3) bonds in Fig. 1. For C2 h symmetry of the Rh-Rh link, . We note that in (1) α and β stand for components in the local, Kitaev bond reference frame. The z axis is here perpendicular to the Rh2O2 plaquette (see SM and refs 14,16,17).
Relative energies for the four low-lying states describing the magnetic spectrum of two NN octahedra and the resulting effective coupling constants are listed in Table 2. For the effective picture of pseudospins assumed in Eq. (1), the set of four eigenfunctions contains the singlet and the triplet components , , . In C2 h symmetry, the “full” spin-orbit wave functions associated to , , and transform according to the Ag, Bu, Bu and Au irreducible representations, respectively. Since two of the triplet terms may interact, the most compact way to express the eigenstates of (1) is then , , and . The angle parametrizes the amount of mixing, related to finite off-diagonal couplings. This degree of admixture is determined by analysis of the full QC spin-orbit wave functions. The effective parameters provided in Table 2 are obtained for each type of Rh-Rh link by using the E1, E2, E3, ES MRCI relative energies and the mixing coefficients (see SM).
For B1 links, we find that both J and K are FM. While by MRCI calculations K always comes FM in spin-orbit coupled honeycomb systems16,17, the FM J for the B1 bonds has much to do with the peculiar kind of dependence on the amount of trigonal squashing of the oxygen octahedra and consequently on the variation of the Rh-O-Rh angles of the Rh2O2 plaquette. The latter increase to values larger than 90° for finite trigonal compression. This dependence of the NN J on the Rh-O-Rh bond angles is illustrated in Fig. 2 for a simplified structural model of Li2RhO3 where the Rh-O bond lengths are all the same, set to the average bond length in the experimental crystal structure33. It is seen that J displays a parabolic behavior, with a minimum of about −5 meV in the interval 92–93° and a change of sign to AF couplings around 96°. For the B1 Rh-Rh links, the Rh-O-Rh bond angle is 93.4°, close to the value that defines the minimum in Fig. 2. The difference between the ≈ − 5 meV minimum of Fig. 2 and the ≈ − 10 meV result listed in Table 2 comes from additional distortions of the O octahedra in the actual structure (see the footnotes in Table 2 and ref. 33), not included in the idealized model considered for the plot in Fig. 2. An even stronger FM J was computed for the B1 type bonds in the related compound Li2IrO317. In Na2IrO3, on the other hand, the Ir-O-Ir bond angles are >97° and the NN J turns AF on all short Ir-Ir links16.
For the B2 and B3 links, we derive a FM Kitaev term and an AF Heisenberg interaction, again qualitatively similar to the QC data for Li2IrO317. We assign the AF value of the NN J on the B2/B3 units to the slightly larger Rh-O-Rh bond angle, which as shown in Fig. 2 pulls the J towards a positive value and most importantly to additional distortions that shift the bridging ligands on the Rh-O2-Rh B2/B3 plaquettes in opposite senses parallel to the Rh-Rh axis33. The role of these additional distortions on the B2/B3 units was analyzed in detail in ref. 16 and shown to enhance as well the AF component to the intersite exchange.
Effect of longer-range exchange interactions and occurence of spin-glass ground state
For further insights into the magnetic properties of Li2RhO3, we carried out ED calculations for an extended spin Hamiltonian that in addition to the NN terms of Eq. (1) incorporates longer-range second- and third-neighbor Heisenberg interactions J2 and J35,7,8,9. We used clusters of 24 sites with periodic boundary conditions4,16,17 and the quantum chemically derived NN coupling constants listed in Table 2. The static spin-structure factor was calculated as function of variable J2 and J3 parameters. For a given set of J2 and J3 values, the dominant order is determined according to the wave number Q = Qmax providing a maximum value of S(Q). The resulting phase diagram is shown in Fig. 3(a). Given the similar structure of the NN magnetic interactions, it is somewhat similar to that obtained in our previous study on Li2IrO317. Six different regions can be identified for meV: FM, Néel, Kitaev spin liquid, stripy, diagonal zigzag and incommensurate Q (ICx) phases. The Kitaev spin liquid, stripy and incommensurate phases in strongly spin-orbit coupled honeycomb 5d5 systems were analyzed in a number of earlier studies4,6,7,8,16. The detailed nature of the diagonal zigzag and incommensurate ICx ground states for large FM J on one set of NN links was described in ref. 17. Remarkably, for J(B1) much larger than K(B1) and J(B2), the initial hexagonal lattice can be mapped onto an effective triangular model of triplet dimers on the B1 bonds17.
Since J2 and J3 are expected to be AF in honeycomb d5 oxides8,9, the most likely candidate for the magnetic ground state of “clean” crystals of Li2RhO3, according to our results, is the diagonal zigzag state (see Fig. 3) and is found to be stable in a wide region of and . Experimentally, however, a spin-glass ground state was determined, with a spin freezing temperature of ~6 K19. As possible cause of the observed spin-glass behavior in Li2RhO3 we here investigate the role of Li-Rh site intercalation. Significant disorder on the cation sublattice is a well known feature in Li2MO3 compounds. A typical value for the degree of Li+ −M4+ site inversion in these materials is 10–15%34,35. Partial substitution of the “in-plane” Rh4+ ions by nonmagnetic Li+ species introduces spin defects in the honeycomb layer. On the 24-site cluster employed for our ED calculations, 10–15% site inversion translates in replacing two centers by vacancies. Hereafter, we denote the two spin defects as p1 and p2.
The effect of spin vacancies on the static spin-structure factor in the diagonal zigzag phase (J2 = J2 = 3) is shown in Fig. 3(d,e). For comparison, the static spin-structure factor is also plotted in Fig. 3(c) for the ideal case without spin defects. In the absence of “defects”, the ground state is characterized in the bulk limit by symmetry-broken long-range order with either or wave vectors. Since the two symmetry-breaking states are degenerate, the structure factor displays four peaks, at Q = Q1 and Q = Q2 [see Fig. 3(c)]. However, by introducing spin vacancies, the degeneracy may be lifted via impurity pinning effects. For example, when the two defects occupy positions 17 and 20 [(p1, p2) = (17, 20), see Fig. 3(b)] the spin structure defines one of the symmetry-breaking states with Q = Q1 [Fig. 3(d)]; likewise, defects at (p1, p2) = (17, 18) yield a state with Q = Q2 [Fig. 3(e)]. In other words, two different kinds of dominant short-range order can be obtained with anti-site disorder. The “locally” favored symmetry-breaking direction depends on the relative positions of the spin vacancies. In a macroscopic system, such “local” domains displaying different symmetry-breaking ordering directions are randomly distributed. Additional frustration is expected to arise because it is not possible to match two differently ordered domains without an emerging “string”. It is therefore likely that by creating some amount of spin defects the long-range zigzag order disappears and the resulting state is perceived as a spin glass at low temperature. A similar mechanism was proposed for the isotropic Heisenberg-Kitaev and J1-J2-J3 models5.
An early well known example of frustration induced through the competition between two different, degenerate spin configurations is the two-dimensional Ising model on a square lattice with randomly distributed, competing FM and AF bonds36. To investigate how the diagonal zigzag state is destroyed by increasing the concentration of spin defects, we also studied a simplified Ising model with J = − ∞ for the B1 bonds, J2 = J3 and all other interactions set to zero. This is a reasonable approximation for the honeycomb layers of Li2RhO3 since the diagonal zigzag phase essentially consists of alternating spin-up and spin-down chains [see sketch in Fig. 3(a)]. Spin structures obtained this way for various spin-defect concentrations x are shown in Fig. 3(f–i). For x = 0 the symmetry-breaking diagonal zigzag state is realized, with degenerate Q = Q1 and Q = Q2 spin structures. At finite, low concentration x ~ 2% those two configurations are no longer degenerate since one of them features slightly lower ground-state energy. We still have in this case a “macroscopically stable” ground state. At intermediate defect concentration x ~ 7% the long-range order is in a strict sense destroyed. However, the large domain walls with either Q = Q1 and Q = Q2 seem to survive. At higher concentration x ~ 12% the long-range order disappears completely. Moreover, we can now identify a mixture of local structures with different symmetry-breaking directions [see Fig. 3(i)].
In sum, we have calculated the microscopic neareast-neighbor magnetic interactions between effective 1/2 spins in Li2RhO3 and uncovered a substantial difference between the two types of bonds that are present: one is dominated by Heisenberg and the other by Kitaev types of couplings. The latter give rise to strong frustration, even if the interactions are predominantly ferromagnetic. In this setting we have additionally considered the effect of the presence of anti-site disorder. Experimentally the in-plane spin-defect concentration in Li2RhO3 has been estimated as x = 10–15%34,35. Based on our theoretical findings it is likely that the observed spin-glass behavior arises from the combination of such anti-site disorder and strongly frustrating magnetic interactions, in particular, the different Kitaev/Heisenberg dominated magnetic bonds and the Ising-like physics associated with the triplet dimer formation that results from there.
Our combined ab initio and effective-model calculations on both Li2RhO3 and related d5 honeycomb iridates16,17,23 indicate that a description in terms of on-site 1/2 pseudospins can well account for the diverse magnetic properties of these systems. While alternative models rely on the formation of delocalized, quasimolecular orbitals37,38 and for Li2RhO3 downplay the role of spin-orbit interactions38, here we show that the latter give rise in Li2RhO3 to anisotropic Kitaev interactions the same magnitude as in 5d iridates16,17,39. That happens in spite of having a Rh t2g splitting δ and a spin-orbit coupling λ of similar magnitude, the same way similar sets of Ir δ and λ parameters in CaIrO340 still generate symmetric anisotropic exchange terms in the range of 10 meV (work is in progress).
The Molpro QC package was employed for all ab initio calculations41. To analyze the electronic ground state and the nature of the d-d excitations, a cluster consisting of one reference RhO6 octahedron plus three NN RhO6 octahedra and 15 nearby Li ions was used. The magnetic spectrum for two Rh4+ ions was obtained from calculations on a cluster containing two reference and four NN RhO6 octahedra plus the surrounding 22 Li ions, see SM for details. The farther solid-state environment was in both cases modeled as a finite array of point charges fitted to reproduce the crystal Madelung field in the cluster region. The spin-orbit treatment was carried out according to the procedure described in ref. 42, using spin-orbit pseudopotentials for Rh.
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We thank V.Yushankhai, Y. Singh, N.A. Bogdanov and U.K. Rößler for useful discussions. L. H. acknowledges financial support from the German Research Foundation (Deutsche Forschungsgemeinschaft, DFG). This work is supported by SFB 1143 of the Deutsche Forschungsgemeinschaft.
The authors declare no competing financial interests.
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Katukuri, V., Nishimoto, S., Rousochatzakis, I. et al. Strong magnetic frustration and anti-site disorder causing spin-glass behavior in honeycomb Li2RhO3. Sci Rep 5, 14718 (2015). https://doi.org/10.1038/srep14718
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