Letter | Published:

Interacting multi-channel topological boundary modes in a quantum Hall valley system

Naturevolume 566pages363367 (2019) | Download Citation

Abstract

Symmetry and topology are central to understanding quantum Hall ferromagnets (QHFMs), two-dimensional electronic phases with spontaneously broken spin or pseudospin symmetry whose wavefunctions also have topological properties1,2. Domain walls between distinct broken-symmetry QHFM phases are predicted to host gapless one-dimensional modes—that is, quantum channels that emerge because of a topological change in the underlying electronic wavefunctions at such interfaces. Although various QHFMs have been identified in different materials3,4,5,6,7,8, interacting electronic modes at these domain walls have not been probed. Here we use a scanning tunnelling microscope to directly visualize the spontaneous formation of boundary modes at domain walls between QHFM phases with different valley polarization (that is, the occupation of equal-energy but quantum mechanically distinct valleys in the electronic structure) on the surface of bismuth. Spectroscopy shows that these modes occur within a topological energy gap, which closes and reopens as the valley polarization switches across the domain wall. By changing the valley flavour and the number of modes at the domain wall, we can realize different regimes in which the valley-polarized channels are either metallic or develop a spectroscopic gap. This behaviour is a consequence of Coulomb interactions constrained by the valley flavour, which determines whether electrons in the topological modes can backscatter, making these channels a unique class of interacting one-dimensional quantum wires. QHFM domain walls can be realized in different classes of two-dimensional materials, providing the opportunity to explore a rich phase space of interactions in these quantum wires.

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The data that support the findings of this study are available from the corresponding author on reasonable request.

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Acknowledgements

The experiments in this project were primarily supported by the Gordon and Betty Moore Foundation as part of the EPiQS initiative (GBMF4530) (B.E.F., H.D., A.Y.) and DOE-BES grant DE-FG02-07ER46419 (M.T.R., A.Y.). Other financial support for the experimental effort came from NSF-DMR-1608848 (A.Y.), NSF-MRSEC programs through the Princeton Center for Complex Materials DMR-142054 (A.Y., R.J.C.) and a Dicke fellowship (B.E.F.). A.Y. acknowledges the hospitality of The Aspen Center for Physics supported under NSF grant PHY-1607611. K.A. acknowledges support from DOE-BES grant no. DE-SC0002140 and from a private bequest to Princeton University by the UK foundation. S.A.P. acknowledges support from NSF DMR-1455366 during the early stages of this project. We acknowledge discussions with S. Kivelson and E. Fradkin.

Reviewer information

Nature thanks Brian LeRoy and the other anonymous reviewer(s) for their contribution to the peer review of this work.

Author information

Author notes

    • Benjamin E. Feldman

    Present address: Geballe Laboratory for Advanced Materials, Stanford University, Stanford, CA, USA

    • Benjamin E. Feldman

    Present address: Department of Physics, Stanford University, Stanford, CA, USA

  1. These authors contributed equally: Mallika T. Randeria, Kartiek Agarwal

Affiliations

  1. Joseph Henry Laboratories and Department of Physics, Princeton University, Princeton, NJ, USA

    • Mallika T. Randeria
    • , Benjamin E. Feldman
    • , Hao Ding
    • , S. L. Sondhi
    •  & Ali Yazdani
  2. Department of Electrical Engineering, Princeton University, Princeton, NJ, USA

    • Kartiek Agarwal
  3. Department of Chemistry, Princeton University, Princeton, NJ, USA

    • Huiwen Ji
    •  & R. J. Cava
  4. The Rudolf Peierls Centre for Theoretical Physics, University of Oxford, Oxford, UK

    • Siddharth A. Parameswaran
  5. Geballe Laboratory for Advanced Materials, Stanford University, Stanford, CA, USA

    • Benjamin E. Feldman
  6. Department of Physics, Stanford University, Stanford, CA, USA

    • Benjamin E. Feldman

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Contributions

M.T.R., B.E.F., H.D. and A.Y. designed and conducted the STM measurements and their analysis. K.A., S.L.S. and S.A.P performed the theoretical calculations. H.J. and R.J.C. synthesized the samples. All authors contributed to the writing of the manuscript.

Competing interests

The authors declare no competing interests.

Corresponding author

Correspondence to Ali Yazdani.

Extended data figures and tables

  1. Extended Data Fig. 1 Role of electron–electron interactions in domain-wall formation.

    a, Spectrum away from the domain wall at B = 13.1 T and T = 250 mK, where the effective filling factor \(\widetilde{\nu }=0\), so the fourfold-degenerate Landau level is not split by exchange. b, Conductance map at the fourfold-degenerate Landau level peak energy E = 700 μeV in the same area as in Fig. 2. The presence of cyclotron orbits of both orientations throughout the image indicates the absence of a domain wall under these conditions. c, Spectroscopic line-cut along the dashed line in b also show a fourfold-degenerate Landau level that does not change across the original location of the domain wall, in stark contrast to the line-cut in Fig. 3a. d, Spectrum away from the domain wall at B = 14 T corresponding to the \(\widetilde{\nu }=2\) domain wall but at a higher temperature of T = 2 K. Again, we do not resolve any exchange splitting, and the Landau level is fourfold degenerate. e, Topography of the same area (identical to Fig. 2d) overlaid with a dI/dV map at E = −100 μeV. We observe cyclotron orbits of both orientations at this increased temperature, and no domain wall is visible. f, Line-cut along the dashed line in e. The absence of splitting in the fourfold-degenerate Landau level confirms that the domain wall is not present at 2 K.

  2. Extended Data Fig. 2 Schematic of strain field and comparison to experimental line-cut.

    a, Schematic of possible strain field (top) and the resulting energies of the different valley states (bottom). A large component of the strain in the direction of valleys C and \(\bar{{\rm{C}}}\) lowers the energy of these two valleys compared with the other four. In the presence of exchange interactions, the switch in strain field from a slight favouring of valleys A and \(\bar{{\rm{A}}}\) to valleys B and \(\bar{{\rm{B}}}\) gives rise to the nematic domain wall. b, Experimental line-cut across the \(\widetilde{\nu }=2\) domain wall showing that the energy of the twofold-degenerate valley state (corresponding to C and \(\bar{{\rm{C}}}\) at E ≈ −1.25 meV) is split off from the other valley states by strain, and does not change substantially across the domain wall associated with the crossing between pairs of valleys (A, \(\bar{{\rm{A}}}\)) and (B, \(\bar{{\rm{B}}}\)) at the Fermi level.

  3. Extended Data Fig. 3 Energy-dependence of the domain-wall behaviour at \(\widetilde{{\boldsymbol{\nu }}}{\bf{=\; 2}}\).

    ai, Differential conductance maps measured in the same location and under identical conditions to those in Fig. 2c. Each panel shows dI/dV at a different energy, ranging from the lower-energy exchange-split Landau level at E = −400 μeV (a) to the higher-energy Landau level peak at E = 400 μeV (i). The data demonstrate the different preferred wavefunction orientations for each respective domain as well as the different orientations of occupied and unoccupied states within a given domain.

  4. Extended Data Fig. 4 Energy-dependence of the domain-wall behaviour at \(\widetilde{{\boldsymbol{\nu }}}{\bf{=\; 1}}\).

    ad, Differential conductance maps measured in the same location and under identical conditions to those in Fig. 2e. Each panel shows dI/dV at a different energy, ranging from the singly degenerate LL at E = −120 μeV (a) to the triply degenerate LL peak at E = 330 μeV (d).

  5. Extended Data Fig. 5 Additional spectroscopic line-cuts across the domain wall.

    af, Spectroscopic line-cuts across the \(\widetilde{\nu }=2\) domain wall. The six different line-cut trajectories are indicated by the dashed lines in m. Although minor variations in the spectra are seen, probably due to the effects of local disorder, the key features of exchange gap closing and Landau level crossing at the domain wall are consistent. gl, Spectroscopic line-cuts across the \(\widetilde{\nu }=1\) domain wall. Again, the same features of the change in topological invariant are present in each line-cut. m, n, dI/dV maps reproduced from Fig. 2c and Fig. 2e, respectively, overlaid with dashed lines showing the locations of the spectroscopic line-cuts in al.

  6. Extended Data Fig. 6 Variation in individual spectra at the domain wall.

    a, Individual spectra (blue, green, brown, purple, black, red) measured for \(\widetilde{\nu }=2\) (a) and \(\widetilde{\nu }=1\) (b), at domain-wall positions corresponding to line 1 to line 6 (Extended Data Fig. 5). All spectra in a show a charge gap Δcharge that is smaller than the exchange gap far from the domain wall (grey dashed spectrum). No Landau level splitting is visible at the \(\widetilde{\nu }=1\) domain wall (b), in contrast to the behaviour in a and far from the domain wall (grey dashed spectrum).

  7. Extended Data Fig. 7 Line-cut along \(\widetilde{{\boldsymbol{\nu }}}{\bf{=\; 2}}\) domain wall.

    a, Line-cut parallel to the \(\widetilde{\nu }=2\) domain wall, along the white line in b, showing spatial variation in the spectra. b, Conductance map reproduced from Fig. 2c, with the location of the spectroscopic line-cut in a marked by the white line.

Supplementary information

  1. Supplementary Information

    This file contains the theoretical modelling of nematic domain-wall behaviour, including Hartree–Fock calculations and modelling of boundary modes using symmetry based Luttinger liquid analysis.

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