pith. sign in

arxiv: 2511.04551 · v2 · submitted 2025-11-06 · ❄️ cond-mat.str-el

High-Temperature Quantum Anomalous Hall Effect in Buckled Honeycomb Antiferromagnets

Mohsen Hafez-Torbati , G\"otz S. Uhrig This is my paper

Pith reviewed 2026-05-18 00:48 UTC · model grok-4.3

classification ❄️ cond-mat.str-el
keywords antiferromagnetic Chern insulatorquantum anomalous Hall effectbuckled honeycomb latticeKondo lattice modelroom-temperature topological phasespin-orbit couplingchiral edge statesNéel antiferromagnet
0
0 comments X

The pith

Buckled honeycomb antiferromagnets become high-temperature antiferromagnetic Chern insulators under a perpendicular electric field.

A machine-rendered reading of the paper's core claim, the machinery that carries it, and where it could break.

The paper proposes that Néel antiferromagnetic Mott insulators on a buckled honeycomb lattice can be driven into an antiferromagnetic Chern insulator phase by a staggered potential from a perpendicular electric field. In a generalized Kondo lattice model the Hall conductance quantizes to e²/h below a temperature set primarily by spin-orbit coupling strength and hopping amplitude. With material parameters typical of heavy transition metals this quantized regime is predicted to extend up to room temperature. The work identifies Sr₃CaOs₂O₉ as a concrete candidate compound and shows that the quantization temperature remains robust across model variations.

Core claim

In the generalized Kondo lattice model of a buckled honeycomb antiferromagnet, the electric-field-induced staggered potential opens a topological gap that converts the Néel Mott insulator into an AF Chern insulator; the Hall conductance stays quantized at e²/h up to a temperature T_q determined essentially by the spin-orbit coupling and hopping parameters, and this T_q reaches room temperature for heavy-transition-metal values.

What carries the argument

Staggered potential generated by a perpendicular electric field acting on the buckled honeycomb lattice, together with antiferromagnetic order and spin-orbit coupling inside the generalized Kondo lattice model, which produces a topological gap, chiral edge states, and quantized Hall conductance.

If this is right

  • The Hall conductance remains quantized up to room temperature for heavy-transition-metal parameters.
  • Chiral edge states develop a finite lifetime and spectral broadening once temperature exceeds the quantization point T_q.
  • Sr₃CaOs₂O₉ is identified as a realizable material platform for the high-temperature AFCI phase.
  • T_q depends mainly on spin-orbit coupling and hopping and is largely insensitive to further model details.

Where Pith is reading between the lines

These are editorial extensions of the paper, not claims the author makes directly.

  • Electric-field tuning of buckling could be tested in other honeycomb lattices to search for similar high-temperature topological phases.
  • Room-temperature operation without external magnetic fields would open pathways for low-dissipation topological transistors.
  • The robustness of T_q across models suggests that first-principles calculations of SOC and hopping in candidate compounds could quickly screen additional materials.

Load-bearing premise

The generalized Kondo lattice model and its temperature evolution of the Hall conductance accurately represent the physics of real buckled honeycomb compounds such as Sr₃CaOs₂O₉.

What would settle it

Measuring the Hall conductance in a thin film of Sr₃CaOs₂O₉ under a perpendicular electric field and finding that quantization to e²/h disappears well below room temperature, or that no chiral edge states appear at all, would falsify the room-temperature prediction.

Figures

Figures reproduced from arXiv: 2511.04551 by G\"otz S. Uhrig, Mohsen Hafez-Torbati.

Figure 1
Figure 1. Figure 1: FIG. 1. (a) Side view of the spin- [PITH_FULL_IMAGE:figures/full_fig_p002_1.png] view at source ↗
Figure 3
Figure 3. Figure 3: FIG. 3. Local magnetizations [PITH_FULL_IMAGE:figures/full_fig_p003_3.png] view at source ↗
Figure 4
Figure 4. Figure 4: FIG. 4. The brick wall representation of the honeycomb structure [PITH_FULL_IMAGE:figures/full_fig_p003_4.png] view at source ↗
Figure 5
Figure 5. Figure 5: FIG. 5. (a) The momentum-resolved spectral function [PITH_FULL_IMAGE:figures/full_fig_p004_5.png] view at source ↗
Figure 6
Figure 6. Figure 6: FIG. 6. Quantization temperature of the Hall conductance vs the [PITH_FULL_IMAGE:figures/full_fig_p004_6.png] view at source ↗
Figure 1
Figure 1. Figure 1: FIG. 1. Position dependence of the local magnetizations [PITH_FULL_IMAGE:figures/full_fig_p007_1.png] view at source ↗
Figure 2
Figure 2. Figure 2: FIG. 2. Schematic comparison of Matsubara and fictitious frequen [PITH_FULL_IMAGE:figures/full_fig_p008_2.png] view at source ↗
Figure 3
Figure 3. Figure 3: FIG. 3. The summand [PITH_FULL_IMAGE:figures/full_fig_p008_3.png] view at source ↗
Figure 5
Figure 5. Figure 5: FIG. 5. (a) Local spectral function vs frequency near the Fermi en [PITH_FULL_IMAGE:figures/full_fig_p009_5.png] view at source ↗
read the original abstract

We propose N\'eel antiferromagnetic (AF) Mott insulators with a buckled honeycomb structure as potential candidates to host a high-temperature AF Chern insulator (AFCI). Using a generalized Kondo lattice model we show that the staggered potential induced by a perpendicular electric field due to the buckling can drive the AF Mott insulator to an AFCI phase. We address the temperature evolution of the Hall conductance and the chiral edge states. The quantization temperature $T_q$, below which the Hall conductance is quantized, depends essentially on the strength of the spin-orbit coupling and the hopping parameter, independent of the specific details of the model. The deviation of the Hall conductance from the quantized value $e^2/h$ above $T_q$ is found to be accompanied by a spectral broadening of the chiral edge states, reflecting a finite life-time, i.e., a decay. Using parameters typical for heavy transition-metal elements we predict that the AFCI can survive up to room temperature. We suggest Sr$_3$CaOs$_2$O$_9$ as a potential compound to realize a high-$T$ AFCI phase.

Editorial analysis

A structured set of objections, weighed in public.

Desk editor's note, referee report, simulated authors' rebuttal, and a circularity audit. Tearing a paper down is the easy half of reading it; the pith above is the substance, this is the friction.

Referee Report

2 major / 1 minor

Summary. The manuscript proposes Néel antiferromagnetic Mott insulators with buckled honeycomb lattices as candidates for high-temperature antiferromagnetic Chern insulators (AFCI). Using a generalized Kondo lattice model, it shows that a perpendicular electric field generates a staggered potential that drives the AF Mott insulator into an AFCI phase. The temperature dependence of the Hall conductance and chiral edge states is analyzed, with the quantization temperature T_q determined essentially by spin-orbit coupling strength and hopping parameter, asserted to be independent of other model details. With parameters typical of heavy transition-metal elements, the AFCI is predicted to survive up to room temperature, and Sr₃CaOs₂O₉ is suggested as a candidate material.

Significance. If the central predictions are robust, the work would be significant for identifying routes to elevated-temperature quantum anomalous Hall effects in antiferromagnetic systems, with potential relevance to topological spintronics. The explicit treatment of finite-temperature evolution of Hall conductance and edge-state lifetime provides a useful addition to the literature on topological phases beyond zero temperature. Credit is due for focusing on a concrete material suggestion and for emphasizing the role of buckling-induced staggered potential.

major comments (2)
  1. [Abstract and model section] Abstract and model section: The central claim that T_q depends essentially on SOC strength and hopping t, independent of specific model details, is demonstrated only within the generalized Kondo lattice model. No explicit comparisons or convergence tests against alternative microscopic Hamiltonians (e.g., Hubbard or t-J models with explicit Néel order and staggered potential) are provided, which directly affects the reliability of the room-temperature prediction for compounds such as Sr₃CaOs₂O₉.
  2. [Material candidate discussion] Material candidate discussion: The room-temperature AFCI prediction relies on 'parameters typical for heavy transition-metal elements' rather than material-specific values or ab-initio calibration for Sr₃CaOs₂O₉. This generic mapping, combined with the single-model assertion of T_q independence, leaves the applicability to real buckled honeycomb compounds unverified.
minor comments (1)
  1. [Abstract] The abstract is somewhat dense; splitting the description of the model, temperature analysis, and material suggestion into clearer sentences would improve readability.

Simulated Author's Rebuttal

2 responses · 0 unresolved

We thank the referee for their positive evaluation of the significance of our work and for the detailed and constructive comments. We address the major comments point by point below, providing clarifications on the scope of our model and predictions while incorporating revisions to improve the manuscript.

read point-by-point responses

  1. Referee: [Abstract and model section] Abstract and model section: The central claim that T_q depends essentially on SOC strength and hopping t, independent of specific model details, is demonstrated only within the generalized Kondo lattice model. No explicit comparisons or convergence tests against alternative microscopic Hamiltonians (e.g., Hubbard or t-J models with explicit Néel order and staggered potential) are provided, which directly affects the reliability of the room-temperature prediction for compounds such as Sr₃CaOs₂O₉.

    Authors: We agree that the explicit demonstration of T_q's dependence on SOC and t is carried out within the generalized Kondo lattice model. This framework was chosen as it captures the essential physics of the Néel AF Mott insulator with SOC while permitting a controlled treatment of the electric-field-induced staggered potential and finite-temperature effects. The asserted independence follows from the effective band structure in which T_q is set by the SOC gap and the hopping scale t after the local moments are integrated out. We acknowledge that direct comparisons to other models such as the Hubbard or t-J Hamiltonian would provide additional support. In the revised manuscript we have added a dedicated paragraph in the model section explaining the rationale for the chosen model, its relation to strong-coupling limits of the Hubbard model, and the expected robustness of the T_q result, while noting that a systematic cross-model study lies beyond the present scope. revision: partial

  2. Referee: [Material candidate discussion] Material candidate discussion: The room-temperature AFCI prediction relies on 'parameters typical for heavy transition-metal elements' rather than material-specific values or ab-initio calibration for Sr₃CaOs₂O₉. This generic mapping, combined with the single-model assertion of T_q independence, leaves the applicability to real buckled honeycomb compounds unverified.

    Authors: The parameters employed are representative values for strong SOC and hopping in 5d transition-metal oxides, drawn from existing literature on related compounds. Sr₃CaOs₂O₉ is suggested as a candidate solely on the basis of its buckled honeycomb lattice and the presence of heavy Os ions. We have revised the material-candidate discussion to cite the sources of the adopted parameter estimates more explicitly, to emphasize that the room-temperature estimate is illustrative, and to state clearly that material-specific ab-initio calculations would be required to refine the parameters and confirm applicability. These changes clarify the proposal nature of the material suggestion without affecting the central theoretical results. revision: yes

Circularity Check

0 steps flagged

Derivation self-contained within single model using external typical parameters

full rationale

The paper constructs a generalized Kondo lattice model for the buckled honeycomb AF Mott insulator, derives the Hall conductance temperature evolution and the quantization temperature T_q explicitly from the model's equations (depending on SOC strength and hopping t), and then inserts externally typical parameter values for heavy transition-metal elements to predict room-temperature survival of the AFCI. No load-bearing step reduces by construction to its own inputs: T_q is computed as an output of the model rather than defined in terms of the target result, the independence from other details is a finding internal to the chosen Hamiltonian, and the high-T claim is a forward prediction from standard parameter ranges rather than a fit or self-referential renaming. The derivation chain is therefore self-contained against external benchmarks and does not exhibit any of the enumerated circularity patterns.

Axiom & Free-Parameter Ledger

2 free parameters · 2 axioms · 0 invented entities

The central claim rests on the validity of the generalized Kondo lattice model for describing the electronic structure of buckled honeycomb AF Mott insulators and on the choice of 'typical' parameter values for heavy transition metals; no new particles or forces are introduced.

free parameters (2)
  • spin-orbit coupling strength
    Controls the size of the topological gap and thus T_q; value taken as typical for heavy TM elements rather than derived.
  • hopping parameter
    Sets the bandwidth and enters the expression for T_q; again taken from typical values.
axioms (2)
  • domain assumption The generalized Kondo lattice model captures the essential low-energy physics of the buckled honeycomb AF Mott insulator.
    Invoked to map the electric-field effect onto an AFCI phase.
  • domain assumption The temperature evolution of the Hall conductance is independent of specific model details beyond SOC and hopping.
    Stated explicitly in the abstract as the basis for the room-temperature prediction.

pith-pipeline@v0.9.0 · 5735 in / 1442 out tokens · 30278 ms · 2026-05-18T00:48:32.154379+00:00 · methodology

discussion (0)

Sign in with ORCID, Apple, or X to comment. Anyone can read and Pith papers without signing in.

Lean theorems connected to this paper

Citations machine-checked in the Pith Canon. Every link opens the source theorem in the public Lean library.

What do these tags mean?
matches
The paper's claim is directly supported by a theorem in the formal canon.
supports
The theorem supports part of the paper's argument, but the paper may add assumptions or extra steps.
extends
The paper goes beyond the formal theorem; the theorem is a base layer rather than the whole result.
uses
The paper appears to rely on the theorem as machinery.
contradicts
The paper's claim conflicts with a theorem or certificate in the canon.
unclear
Pith found a possible connection, but the passage is too broad, indirect, or ambiguous to say the theorem truly supports the claim.

Reference graph

Works this paper leans on

76 extracted references · 76 canonical work pages

  1. [1]

    where c† iα is the fermion creation operator at the site i with the z-component of the spin α =↑ or ↓

    illustrated in (b) for the special case of Stot = 3/ 2. where c† iα is the fermion creation operator at the site i with the z-component of the spin α =↑ or ↓. The first term is the NN hopping and the second term is the Hund coupling be- tween the electron spin ⃗ si and the localized spin ⃗Si with the spin quantum number S = Stot − 1/ 2. We treat one orbita...

    work page

  2. [2]

    We al- ways count the Heisenberg interaction on each lattice bond only once

    is the Hubbard interaction with niα := c† iα ciα , and the fourth term is the Heisenberg interaction between the NN spins. We al- ways count the Heisenberg interaction on each lattice bond only once. The fifth term is the staggered sublattice potential giving the onsite energies +δ and − δ to the two sublattices of the honeycomb structure. Figure 1(b) illu...

    work page

  3. [3]

    to J = 4 t2/ ∆ 0 with ∆ 0 := U + 2SJH, called the bare Mott gap. This guarantees the Heisenberg model ( 1) as the low-energy effective model of the Hamiltonian ( 2) for δ = 0 , apart from some weak anisotropic interactions origi- nating from the spin-orbit coupling λ SO. The Hamiltonian ( 2) generalizes the purely spin model ( 1) allowing for the study of...

    work page

  4. [4]

    at finite temperature are rare. We employ the dynamical mean-field theory (DMFT) [ 28] as an established method for strongly correlated systems and use the exact di- agonalization (ED) as the impurity solver [ 28, 29]. We specif- ically use the real-space realization of the DMFT [ 30] provid- ing access to the bulk and the edge properties on equal footing [...

    work page

  5. [5]

    ( 1), see Fig

    corresponds to the total spin Stot = 1 in Eq. ( 1), see Fig. 1. The number of bath sites nb = 5 is used in the ED. The colormap displays the value of the Hall conductance σ yx = − σ xy. The Néel temperature TN and the crossover quantization temperature Tq are specified. The Hall conductance acquires the quantized value e2/h with an error less than %1 below...

    work page

  6. [6]

    corresponds to the total spin Stot = S + 1/ 2 = 1 in Eq. ( 1). The number of bath sites nb = 5 is used in the ED impurity solver. [ 32, 35]. Thus, the itinerant electrons are in the band insulator phase above TN. The intermediate values of δ are of particular interest be- cause the Hall conductance becomes non-zero and approaches the quantized value e2/h ...

    work page

  7. [7]

    We consider Nx = 80

    At each x, there are two nonequivalent lattice sites in the y direction. We consider Nx = 80. The momentum-resolved spectral function A↑,x =0(ω, k y), averaged over the two nonequivalent lattice sites in the y di- rection, is plotted in Fig. 5(a) for the same model param- eters as in Fig. 3. The results are for the topological spin component α =↑. The spi...

    work page

  8. [8]

    3 Å [ 41], respectively

    3 Å [ 39, 40] and 3. 3 Å [ 41], respectively. The latter com- pound shows a Néel AF order with the high Néel temperature TN ∼ 385 K and is a promising candidate to host a high- T AFCI. Growing [111]-oriented bilayers of perovskite heavy transition-metal oxides is another route to a buckled honey- comb antiferromagnet [ 42] and a high- T AFCI state. Our fin...

    work page

  9. [9]

    Chang, C.-X

    C.-Z. Chang, C.-X. Liu, and A. H. MacDonald, Colloquium: Quantum anomalous Hall effect, Rev. Mod. Phys. 95, 011002 (2023)

    work page 2023

  10. [10]

    Tokura, K

    Y . Tokura, K. Y asuda, and A. Tsukazaki, Magnetic topological insulators, Nature Reviews Physics 1, 126 (2019)

    work page 2019

  11. [11]

    Chang, J

    C.-Z. Chang, J. Zhang, X. Feng, J. Shen, Z. Zhang, M. Guo, K. Li, Y . Ou, P . Wei, L.-L. Wang, Z.-Q. Ji, Y . Feng, S. Ji, X. Chen, J. Jia, X. Dai, Z. Fang, S.-C. Zhang, K. He, Y . Wang, L. Lu, X.-C. Ma, and Q.-K. Xue, Experimental Observation of the Quantum Anomalous Hall Effect in a Magnetic Topological Insulator, Science 340, 167 (2013)

    work page 2013

  12. [12]

    Chang, W

    C.-Z. Chang, W. Zhao, D. Y . Kim, H. Zhang, B. A. Assaf, D. Heiman, S.-C. Zhang, C. Liu, M. H. W. Chan, and J. S. Moodera, High-precision realization of robust quantum anoma- lous Hall state in a hard ferromagnetic topological insulator, Nature Materials 14, 473 (2015)

    work page 2015

  13. [13]

    M. Mogi, R. Y oshimi, A. Tsukazaki, K. Y asuda, Y . Kozuka, K. S. Takahashi, M. Kawasaki, and Y . Tokura, Magnetic modulation doping in topological insulators toward higher- temperature quantum anomalous Hall effect, Applied Physics Letters 107, 182401 (2015)

    work page 2015

  14. [14]

    J. Zhu, Y . Feng, X. Zhou, Y . Wang, H. Y ao, Z. Lian, W. Lin, Q. He, Y . Lin, Y . Wang, Y . Wang, S. Y ang, H. Li, Y . Wu, C. Liu, J. Wang, J. Shen, J. Zhang, Y . Wang, and Y . Wang, Direct obser- vation of chiral edge current at zero magnetic field in a magnetic topological insulator, Nature Communications 16, 963 (2025)

    work page 2025

  15. [15]

    Y . Deng, Y . Y u, M. Z. Shi, Z. Guo, Z. Xu, J. Wang, X. H. Chen, and Y . Zhang, Quantum anomalous Hall effect in intrinsic mag- netic topological insulator MnBi2Te4, Science 367, 895 (2020)

    work page 2020

  16. [16]

    C. Liu, Y . Wang, H. Li, Y . Wu, Y . Li, J. Li, K. He, Y . Xu, J. Zhang, and Y . Wang, Robust axion insulator and Chern insu- lator phases in a two-dimensional antiferromagnetic topological insulator, Nature Materials 19, 522 (2020)

    work page 2020

  17. [17]

    T. Li, S. Jiang, B. Shen, Y . Zhang, L. Li, Z. Tao, T. Devakul, K. Watanabe, T. Taniguchi, L. Fu, J. Shan, and K. F. Mak, Quantum anomalous Hall effect from intertwined moiré bands, Nature 600, 641 (2021)

    work page 2021

  18. [18]

    Serlin, C

    M. Serlin, C. L. Tschirhart, H. Polshyn, Y . Zhang, J. Zhu, K. Watanabe, T. Taniguchi, L. Balents, and A. F. Y oung, Intrin- sic quantized anomalous Hall effect in a moiré heterostructure, Science 367, 900 (2020)

    work page 2020

  19. [19]

    Baltz, A

    V . Baltz, A. Manchon, M. Tsoi, T. Moriyama, T. Ono, and Y . Tserkovnyak, Antiferromagnetic spintronics, Rev. Mod. Phys. 90, 015005 (2018)

    work page 2018

  20. [22]

    Bossini, M

    D. Bossini, M. Terschanski, F. Mertens, G. Springholz, A. Bo- nanni, G. S. Uhrig, and M. Cinchetti, Exchange-mediated mag- netic blue-shift of the band-gap energy in the antiferromag- netic semiconductor MnTe, New Journal of Physics 22, 083029 (2020)

    work page 2020

  21. [23]

    Sangiovanni, A

    G. Sangiovanni, A. Toschi, E. Koch, K. Held, M. Capone, C. Castellani, O. Gunnarsson, S.-K. Mo, J. W. Allen, H.-D. Kim, A. Sekiyama, A. Y amasaki, S. Suga, and P . Metcalf, Static versus dynamical mean-field theory of Mott antiferromagnets, Phys. Rev. B 73, 205121 (2006)

    work page 2006

  22. [24]

    Y .-J. Hao, P . Liu, Y . Feng, X.-M. Ma, E. F. Schwier, M. Arita, S. Kumar, C. Hu, R. Lu, M. Zeng, Y . Wang, Z. Hao, H.-Y . Sun, K. Zhang, J. Mei, N. Ni, L. Wu, K. Shimada, C. Chen, Q. Liu, and C. Liu, Gapless Surface Dirac Cone in Antifer- romagnetic Topological Insulator MnBi 2Te4, Phys. Rev. X 9, 041038 (2019)

    work page 2019

  23. [25]

    Y . J. Chen, L. X. Xu, J. H. Li, Y . W. Li, H. Y . Wang, C. F. Zhang, H. Li, Y . Wu, A. J. Liang, C. Chen, S. W. Jung, C. Cacho, Y . H. Mao, S. Liu, M. X. Wang, Y . F. Guo, Y . Xu, Z. K. Liu, L. X. Y ang, and Y . L. Chen, Topological Electronic Structure and Its Temperature Evolution in Antiferromagnetic Topological Insu- lator MnBi2Te4, Phys. Rev. X 9, 0...

    work page 2019

  24. [26]

    Li, S.-Y

    H. Li, S.-Y . Gao, S.-F. Duan, Y .-F. Xu, K.-J. Zhu, S.-J. Tian, J.-C. Gao, W.-H. Fan, Z.-C. Rao, J.-R. Huang, J.-J. Li, D.-Y . Y an, Z.-T. Liu, W.-L. Liu, Y .-B. Huang, Y .-L. Li, Y . Liu, G.- B. Zhang, P . Zhang, T. Kondo, S. Shin, H.-C. Lei, Y .-G. Shi, W.-T. Zhang, H.-M. Weng, T. Qian, and H. Ding, Dirac Surface States in Intrinsic Magnetic Topologica...

    work page 2019

  25. [27]

    Swatek, Y

    P . Swatek, Y . Wu, L.-L. Wang, K. Lee, B. Schrunk, J. Y an, and A. Kaminski, Gapless Dirac surface states in the antifer- romagnetic topological insulator MnBi 2Te4, Phys. Rev. B 101, 161109 (2020)

    work page 2020

  26. [28]

    Jiang, S

    K. Jiang, S. Zhou, X. Dai, and Z. Wang, Antiferromagnetic Chern Insulators in Noncentrosymmetric Systems, Phys. Rev. Lett. 120, 157205 (2018)

    work page 2018

  27. [29]

    Ebrahimkhas, G

    M. Ebrahimkhas, G. S. Uhrig, W. Hofstetter, and M. Hafez- Torbati, Antiferromagnetic Chern insulator in centrosymmetric systems, Phys. Rev. B 106, 205107 (2022)

    work page 2022

  28. [30]

    Guo, Z.-X

    P .-J. Guo, Z.-X. Liu, and Z.-Y . Lu, Quantum anomalous Hall effect in collinear antiferromagnetism, npj Computational Ma- terials 9, 70 (2023)

    work page 2023

  29. [31]

    Hafez-Torbati, Antiferromagnetic topological insulators in heavy-fermion systems, Phys

    M. Hafez-Torbati, Antiferromagnetic topological insulators in heavy-fermion systems, Phys. Rev. B 110, 115147 (2024)

    work page 2024

  30. [32]

    Hafez-Torbati and G

    M. Hafez-Torbati and G. S. Uhrig, Antiferromagnetic chern in- sulator with large charge gap in heavy transition-metal com- pounds, Scientific Reports 14, 17168 (2024)

    work page 2024

  31. [33]

    Wu, Y .-l

    B. Wu, Y .-l. Song, W.-x. Ji, P .-j. Wang, S.-f. Zhang, and C.-w. Zhang, Quantum anomalous Hall effect in an antiferromagnetic monolayer of MoO, Phys. Rev. B 107, 214419 (2023)

    work page 2023

  32. [34]

    Fazekas, Lecture Notes on Electron Correlation and Mag- netism, Series in modern condensed matter physics (World Sci- entific, 1999)

    P . Fazekas, Lecture Notes on Electron Correlation and Mag- netism, Series in modern condensed matter physics (World Sci- entific, 1999)

    work page 1999

  33. [35]

    C. L. Kane and E. J. Mele, Quantum Spin Hall Effect in Graphene, Phys. Rev. Lett. 95, 226801 (2005)

    work page 2005

  34. [36]

    Georges, G

    A. Georges, G. Kotliar, W. Krauth, and M. J. Rozenberg, Dy- namical mean-field theory of strongly correlated fermion sys- tems and the limit of infinite dimensions, Rev. Mod. Phys. 68, 13 (1996)

    work page 1996

  35. [37]

    Caffarel and W

    M. Caffarel and W. Krauth, Exact diagonalization approach to correlated fermions in infinite dimensions: Mott transition and superconductivity, Phys. Rev. Lett. 72, 1545 (1994)

    work page 1994

  36. [40]

    (2), for the analysis of the Hall conductance in Eq

    See Supplemental Materials for the DMFT solution of Eq. (2), for the analysis of the Hall conductance in Eq. (3), for the calcu- lation of the spectral function on the cylindrical geometry, and for further details of the phase diagram in Fig. 2

    work page

  37. [41]

    Ishikawa and T

    K. Ishikawa and T. Matsuyama, A microscopic theory of the 6 quantum Hall effect, Nuclear Physics B 280, 523 (1987)

    work page 1987

  38. [42]

    Manousakis, The Spin- 1 2 Heisenberg Antiferromanget on a Square Lattice and its Application to the Cuprous Oxides, Rev

    E. Manousakis, The Spin- 1 2 Heisenberg Antiferromanget on a Square Lattice and its Application to the Cuprous Oxides, Rev. Mod. Phys. 63, 1 (1991)

    work page 1991

  39. [43]

    J. H. V an Vleck, The Theory of Electric and Magnetic Suscep- tibilities (Oxford University Press, 1932)

    work page 1932

  40. [44]

    Z. Ni, Q. Liu, K. Tang, J. Zheng, J. Zhou, R. Qin, Z. Gao, D. Y u, and J. Lu, Tunable bandgap in silicene and germanene, Nano Lett. 12, 113 (2012)

    work page 2012

  41. [45]

    Zhang, T.-T

    Y . Zhang, T.-T. Tang, C. Girit, Z. Hao, M. C. Martin, A. Zettl, M. F. Crommie, Y . R. Shen, and F. Wang, Direct observation of a widely tunable bandgap in bilayer graphene, Nature 459, 820 (2009)

    work page 2009

  42. [46]

    Sakanashi, N

    K. Sakanashi, N. Wada, K. Murase, K. Oto, G.-H. Kim, K. Watanabe, T. Taniguchi, J. P . Bird, D. K. Ferry, and N. Aoki, V alley polarized conductance quantization in bilayer graphene narrow quantum point contact, Applied Physics Letters 118, 263102 (2021)

    work page 2021

  43. [47]

    S. Asai, M. Soda, K. Kasatani, T. Ono, M. Avdeev, and T. Ma- suda, Magnetic ordering of the buckled honeycomb lattice anti- ferromagnet Ba2NiTeO6, Phys. Rev. B 93, 024412 (2016)

    work page 2016

  44. [48]

    S. Asai, M. Soda, K. Kasatani, T. Ono, V . O. Garlea, B. Winn, and T. Masuda, Spin dynamics in the stripe-ordered buckled honeycomb lattice antiferromagnet Ba 2NiTeO6, Phys. Rev. B 96, 104414 (2017)

    work page 2017

  45. [49]

    G. S. Thakur, T. C. Hansen, W. Schnelle, S. Guo, O. Janson, J. van den Brink, C. Felser, and M. Jansen, Buckled honeycomb lattice compound Sr 3CaOs2O9 exhibiting antiferromagnetism above room temperature, Chem. Mater. 34, 4741 (2022)

    work page 2022

  46. [50]

    D. Xiao, W. Zhu, Y . Ran, N. Nagaosa, and S. Okamoto, Inter- face engineering of quantum Hall effects in digital transition metal oxide heterostructures, Nature Communications 2, 596 (2011). Supplemental Material: High-Temperature Quantum Anomalous Hall Effect in Buckled Honeycomb Antiferromagnets Mohsen Hafez-Torbati 1, ∗ and Götz S. Uhrig 2, † 1Departme...

    work page 2011

  47. [51]

    To study the system with the cylindrical geometry we fix the expecta- tion values ⟨Sz i ⟩ and ⟨sz i ⟩ in Eq

    is justified for the cylindrical geometry because the edge effects on ⟨Sz i ⟩ and ⟨sz i ⟩ is extremely small. To study the system with the cylindrical geometry we fix the expecta- tion values ⟨Sz i ⟩ and ⟨sz i ⟩ in Eq. (

    work page

  48. [52]

    This fixes the Hamiltonian and avoids too many unknown parameters, which allows for an easier and faster convergence of the DMFT loop [ 8]

    to what we have already found for the bulk, using the periodic boundary conditions in both directions. This fixes the Hamiltonian and avoids too many unknown parameters, which allows for an easier and faster convergence of the DMFT loop [ 8]. Note that for the cylindrical geometry, the impurity model at each DMFT iter- ation has to be set up and solved for...

    work page

  49. [53]

    for the cylindrical geometry. II. HALL CONDUCTANCE The topological invariant form of the Hall conductance σ xy in Eq. (3) in the main text can be simplified to σ xy = ∑ α σ α xy = ∑ α ∑ n S α xy(iω n) , (2a) S α xy(iω n) = e2 h T 2π Re [∫ d⃗k Tr [ Gα ∂kyH(0) α × ∂ω nGα ∂kxH(0) α ] ] (2b) where we have used the facts that the conductance is an an- tisymmetr...

    work page

  50. [54]

    and ∂ω n Gα ≡ ∂ω Gα (iω, ⃗k)|ω =ω n

    to compute the derivative of the Green’s function at a Mat- subara frequency. and ∂ω n Gα ≡ ∂ω Gα (iω, ⃗k)|ω =ω n . The Bloch Hamiltonian matrix and its derivatives in Eq. ( 2b) can be calculated analyt- ically. The Green’s function can also be rigorously evaluated at different frequencies using the self-energy obtained from the DMFT. What is somewhat cha...

    work page

  51. [55]

    The fictitious frequency ω fic n , at which the derivative is calculated, is assumed to match a Matsubara frequency

    To accurately estimate the derivative of the Green’s function at the Matsubara frequencies we use the five-point central difference formula, ∂ω G(iω ) ⏐ ⏐ ω =ω fic n = 1 24πT fic ( G(iω fic n− 2) + 8G(iω fic n+1) − 8G(iω fic n− 1) − G(iω fic n+2) ) (3) where we have dropped the spin α and the momentum ⃗k de- pendence of the Green’s function to lighten the notat...

    work page

  52. [56]

    2 for Tfic = T / 5

    to compute the derivative of the Green’s function at a Matsubara frequency are distinguished by an un- der bracket in Fig. 2 for Tfic = T / 5. We have mainly used Tfic = T / 5 in the calculations. Nevertheless, for selective points close to the phase transitions we have checked that the results accurately match the results obtained for Tfic = T / 3 and T / 7...

    work page

  53. [57]

    9992, respectively, for Tfic = T , T / 3, T / 5, and T / 7

    9991, and 0. 9992, respectively, for Tfic = T , T / 3, T / 5, and T / 7. It is interesting to see how the summand in Eq. ( 2) changes across a topological phase transition, where the Hall conduc- tance abruptly jumps between 0 and e2/h . We consider the topological phase transition at δc1 ≃ 6. 2t at the low tempera- ture T = 0 . 02t in Fig. 2 in the main t...

    work page

  54. [58]

    The topological properties of an interacting system at zero temperature can be determined via an effective non-interacting model known as the topological Hamiltonian

    at low temperatures. The topological properties of an interacting system at zero temperature can be determined via an effective non-interacting model known as the topological Hamiltonian. Definitely, the method has some limitations. For example, it holds for fermionic systems at T = 0 and cannot be applied to bosonic bands [ 12]. The topological Hamiltonia...

    work page

  55. [59]

    at low temperatures 3 (c) charge gap δ/t α=↑ α=↓ 0.0 1.0 2.0 3.0 4.0 5.0 6.0 5 6 7 8 9 α (b) σyx [e2/h] α=↑ α=↓ 0.0 0.2 0.4 0.6 0.8 1.0 (a) expectation values M m K 0.0 0.1 0.2 0.3 0.4 0.5 δ=8.6t Aα(ω)t ω/t 0.0 0.2 0.4 0.6 -4 -3 -2 -1 0 1 2 3 4 δ=8.2t Aα(ω)t 0.0 0.2 0.4 0.6 δ=7.8t Aα(ω)t 0.0 0.2 0.4 0.6 δ=6.6t Aα(ω)t 0.0 0.2 0.4 0.6 δ=6.2t Aα(ω)t 0.0 0.2 ...

    work page

  56. [60]

    We attribute the small deviation to the finite spin-orbit coupling in Fig

    5¯ 5t with the coordination number Z = 3 . We attribute the small deviation to the finite spin-orbit coupling in Fig. 2 in the main text. For large values of δ the magnetic properties of the system is mainly due to the localized spins. The itinerant electrons show a very weak magnetization. The Néel temper- ature for large values of δ in Fig. 2 in the main...

    work page

  57. [61]

    2U , J = 4 t2/ ∆ 0 = 0

    The results are for S = 1 / 2, U = 12 t, JH = 0 . 2U , J = 4 t2/ ∆ 0 = 0 . 2¯ 7t, and λ SO = 0 . 2t (the same model 4 parameters as in Fig. 2 in the main text) at the temperature T = 0. 6t. The number of bath sites nb = 6 is used in the ED impurity solver. Fig. 5(a) displays the local spectral function vs frequency near the Fermi energy ω = 0 for differen...

    work page

  58. [62]

    The momentum-resolved spectral function Aα, ⃗d (ω, k y) for the spin component α at the lattice site ⃗d = ( x, y ) in the unit cell is then easily obtained via Eq

    and the DMFT self-energy Σ α (ω + i η). The momentum-resolved spectral function Aα, ⃗d (ω, k y) for the spin component α at the lattice site ⃗d = ( x, y ) in the unit cell is then easily obtained via Eq. 4 in the main text. We have used the broadening factor η = 0. 01t as mentioned in the main text

    work page

  59. [63]

    Potthoff and W

    M. Potthoff and W. Nolting, Surface metal-insulator transition in the Hubbard model, Phys. Rev. B 59, 2549 (1999)

    work page 1999

  60. [64]

    Y . Song, R. Wortis, and W. A. Atkinson, Dynamical mean field study of the two-dimensional disordered Hubbard model, Phys. Rev. B 77, 054202 (2008)

    work page 2008

  61. [65]

    Snoek, I

    M. Snoek, I. Titvinidze, C. T ˝oke, K. Byczuk, and W. Hofstetter, Antiferromagnetic order of strongly interacting fermions in a trap: real-space dynamical mean-field analysis, New Journal of Physics 10, 093008 (2008)

    work page 2008

  62. [66]

    Hafez-Torbati and W

    M. Hafez-Torbati and W. Hofstetter, Artificial SU(3) spin-orbit coupling and exotic Mott insulators, Phys. Rev. B 98, 245131 (2018)

    work page 2018

  63. [67]

    Hafez-Torbati, F

    M. Hafez-Torbati, F. B. Anders, and G. S. Uhrig, Simplified approach to the magnetic blue shift of Mott gaps, Phys. Rev. B 106, 205117 (2022)

    work page 2022

  64. [68]

    Hafez-Torbati, D

    M. Hafez-Torbati, D. Bossini, F. B. Anders, and G. S. Uhrig, Magnetic blue shift of Mott gaps enhanced by double exchange, Phys. Rev. Research 3, 043232 (2021)

    work page 2021

  65. [69]

    Müller-Hartmann, Correlated fermions on a lattice in high dimensions, Zeitschrift für Physik B Condensed Matter 74, 507 (1989)

    E. Müller-Hartmann, Correlated fermions on a lattice in high dimensions, Zeitschrift für Physik B Condensed Matter 74, 507 (1989)

    work page 1989

  66. [70]

    Hafez-Torbati, From explicit to spontaneous charge order and the fate of the antiferromagnetic quantum Hall state, Phys

    M. Hafez-Torbati, From explicit to spontaneous charge order and the fate of the antiferromagnetic quantum Hall state, Phys. Rev. B 111, 125108 (2025)

    work page 2025

  67. [71]

    Y oshida, S

    T. Y oshida, S. Fujimoto, and N. Kawakami, Correlation effects on a topological insulator at finite temperatures, Phys. Rev. B 5 85, 125113 (2012)

    work page 2012

  68. [72]

    Irsigler, T

    B. Irsigler, T. Grass, J.-H. Zheng, M. Barbier, and W. Hofstetter, Topological Mott transition in a Weyl-Hubbard model: Dynam- ical mean-field theory study, Phys. Rev. B 103, 125132 (2021)

    work page 2021

  69. [73]

    Wang and S.-C

    Z. Wang and S.-C. Zhang, Simplified Topological Invariants for Interacting Insulators, Phys. Rev. X 2, 031008 (2012)

    work page 2012

  70. [74]

    Hawashin, J

    B. Hawashin, J. Sirker, and G. S. Uhrig, Topological proper- ties of single-particle states decaying into a continuum due to interaction, Phys. Rev. Res. 6, L042041 (2024)

    work page 2024

  71. [75]

    Hafez-Torbati and G

    M. Hafez-Torbati and G. S. Uhrig, Antiferromagnetic Chern in- sulator with large charge gap in heavy transition-metal com- pounds, Scientific Reports 14, 17168 (2024)

    work page 2024

  72. [76]

    A. Garg, H. R. Krishnamurthy, and M. Randeria, Can Corre- lations Drive a Band Insulator Metallic?, Phys. Rev. Lett. 97, 046403 (2006)

    work page 2006

  73. [77]

    Paris, K

    N. Paris, K. Bouadim, F. Hébert, G. G. Batrouni, and R. T. Scalettar, Quantum Monte Carlo Study of an Interaction- Driven Band-Insulator-to-Metal Transition, Phys. Rev. Lett. 98, 046403 (2007)

    work page 2007

  74. [78]

    Byczuk, M

    K. Byczuk, M. Sekania, W. Hofstetter, and A. P . Kampf, Insu- lating behavior with spin and charge order in the ionic Hubbard model, Phys. Rev. B 79, 121103 (2009)

    work page 2009

  75. [79]

    S. S. Kancharla and E. Dagotto, Correlated Insulated Phase Suggests Bond Order between Band and Mott Insulators in Two Dimensions, Phys. Rev. Lett. 98, 016402 (2007)

    work page 2007

  76. [80]

    Hafez-Torbati and G

    M. Hafez-Torbati and G. S. Uhrig, Orientational bond and Néel order in the two-dimensional ionic Hubbard model, Phys. Rev. B 93, 195128 (2016)

    work page 2016