Abstract
It has recently been shown that electronic states in bulk gapless HgCdTe offer another realization of pseudorelativistic threedimensional particles in condensed matter systems. These single valley relativistic states, massless Kane fermions, cannot be described by any other relativistic particles. Furthermore, the HgCdTe band structure can be continuously tailored by modifying cadmium content or temperature. At critical concentration or temperature, the bandgap collapses as the system undergoes a semimetaltosemiconductor topological phase transition between the inverted and normal alignments. Here, using farinfrared magnetospectroscopy we explore the continuous evolution of band structure of bulk HgCdTe as temperature is tuned across the topological phase transition. We demonstrate that the rest mass of Kane fermions changes sign at critical temperature, whereas their velocity remains constant. The velocity universal value of (1.07±0.05) × 10^{6} m s^{−1} remains valid in a broad range of temperatures and Cd concentrations, indicating a striking universality of the pseudorelativistic description of the Kane fermions in HgCdTe.
Introduction
In condensed matter systems, the interaction of electrons with a periodic crystal lattice potential can give rise to lowenergy quasiparticles that mimic the relativistic dynamics of Dirac particles in highenergy physics. Perhaps the most spectacular demonstration of this concept was given ten years ago by the isolation of a monolayer of carbon atoms forming a graphene^{1} sheet. The electrons in graphene behave as twodimensional (2D) massless fermions with gapless conical bands that obey the Dirac equation. Subsequently, further condensed matter analogues of highenergy relativistic fermions were demonstrated such as edge or surface states of 2D or threedimesnional (3D) topological insulators^{2,3,4} and 3D Dirac semimetals with linear energymomentum dispersion in all three momentum directions^{5,6,7}.
Recently, another massless Diraclike quasiparticle has been discovered in Hg_{1−x}Cd_{x}Te at an invertedtonormal band structure topological transition existing at the critical cadmium concentration^{8} x_{C}≈0.17. These 3D massless Kane fermions are not equivalent to any other known relativistic particles. Similar to the pseudospin1 Dirac–Weyl system^{9}, their energy dispersion relation features cones crossed at the vertex by an additional flat band. The bandgap and the electronic dispersion in Hg_{1−x}Cd_{x}Te can be tuned intrinsically by adjusting the chemical composition, or externally, by changing temperature^{10}. The ability to control the properties of quasiparticles with relativistic behaviour in a tabletop condensedmatter experiment holds vast scientific and technological potential. However, the variation of the chemical composition in Hg_{1−x}Cd_{x}Te crystals does not allow for finetuning of the bandgap in the vicinity of the phase transition due to inherent fluctuations of Cd concentration. Contrarily, a temperaturedriven evolution of the band structure (see also Supplementary Note 1) provides a conceptually straightforward, yet very accurate and detailed probe of the relativistic properties of Kane fermions, while tuning the 3D Hg_{1−x}Cd_{x}Te across the gapless state at the topological transition between a normal state and an inverted bandgap state. The appearance of a nonzero gap does not exclude relativistic properties of the Kane fermions in Hg_{1−x}Cd_{x}Te, which is retained at energies significantly above the gap. The energy dispersion asymptotically tends to a linear behaviour, as it is for relativistic electrons at high energies. The cutoff energies for relativistic behaviour in the Hg_{1−x}Cd_{x}Te compounds and in other 3D Dirac–Weyl semimetals are related to the presence of highlying conduction bands and lowlying valence bands.
Here we conduct a systematic optical investigation of the dispersion of Kane fermions in Hg_{1−x}Cd_{x}Te crystal as a function of temperature and magnetic field. From the experimental point of view, the use of temperature as a band structure tuning parameter in magnetooptical studies is challenging and demands ultimate quality samples. This is because the observation of welldefined optical resonances requires high carrier mobility, which degrades with increasing temperature due to the increase of scattering on phonons. Our bulk Hg_{1−x}Cd_{x}Te samples were grown by molecular beam epitaxy. The Cd concentration was chosen to enable exploring the bandgap E_{g}(x, T) space across the semimetaltosemiconductor phase transition using temperature for fine gapatwill tuning. The sample A, x=0.175, is a standard narrowgap semiconductor at any temperature. The sample B, x=0.155, is a semimetal at low temperatures with a negative bandgap corresponding to the inverted band order. As the temperature increases, the inverted bandgap closes as the system undergoes a semimetaltosemiconductor phase transition at the critical temperature T_{C}≈77 K followed by the opening of a gap in the normal state. Based on a simplified Kane model, we determine the Kane fermions velocity and rest mass. The rest mass experiences a change of sign at the critical temperature of topological phase transition. Our study reveals a universal velocity of 1.07 × 10^{6} m s^{−1} in HgTe crystals. This further allows to determine the Kane fermion rest mass from all experimental results, past or future, close to the phase transition.
Results
Band structure evolution with temperature
To describe the electronic structure near the centre of the Brillouin zone in Hg_{1−x}Cd_{x}Te close to x_{C}, we employ a simplified Kane model^{11,12} taking into account k·p interaction between the Γ_{6} and Γ_{8} bands, while neglecting the influence of the splitoff Γ_{7} band. The corresponding (6 × 6) Hamiltonian formally resembles the one for relativistic 3D Dirac particles (see ‘Simplified Kane model’ in Methods). By neglecting small quadratic in momentum terms, the eigenvalues of this Hamiltonian can be presented in the form:
The first eigenvalue ξ=0 corresponds to the flat heavyhole band. The two other eigenvalues describe the electron (ξ=+1) and lighthole (ξ=−1) conical bands separated by is a Heaviside step function, which equals to 1 for and to 0 if is negative. This representation of Kane fermions in Hg_{1−x}Cd_{x}Te contains only two parameters, the rest mass and the universal velocity , whereas the material properties are introduced through the Kane’s matrix element P and the Hg_{1−x}Cd_{x}Te bandgap E_{g}.
The evolution of Kane fermions in Hg_{1−x}Cd_{x}Te is illustrated in Fig. 1. If the rest mass is positive, the crystal is a typical narrowgap semiconductor with the stype Γ_{6} band lying above the ptype Γ_{8} bands, as schematically shown on Fig. 1a. On the other hand, if <0, the band order is inverted: the Γ_{6} band lies below the Γ_{8} bands. As the two Γ_{8} bands always touch each other at the Γ point of the Brillouin zone, the band structure is gapless and the crystal is a semimetal. The two distinct phases with different sign of the rest mass are not topologically equivalent, as characterized by a Z_{2} topological invariant^{13}.
Experimentally, the dispersion of gapless or gapped 2D or 3D Dirac fermions can be conveniently probed through the magnetic field dependence of interLandau level transitions^{14,15,16,17,18,19,20}. The application of a quantizing magnetic field B transforms the zerofield continuum of states into a set of unequally spaced Landau levels (LLs) with a distinct behaviour. In pristine gapless graphene, for example, the LLs have a simple structure given by^{14}: , where ħ is the Planck constant and e is the electron charge. The integer LL index n labels electron (n>0) and holelike (n<0) states, and unconventional, zeroenergy fieldindependent n=0 LL states. In graphene/boronnitride heterostructures with zero crystallographic alignment angle, an intrinsic gap Δ opens up separating zeroth dispersionless LLs, E_{n=0}=±Δ/2. Other n>0 electron(hole)like LLs shift up(down) by Δ/2 as well: (after ref. 17).
The LL spectrum of massive or massless fermions in Hg_{1−x}Cd_{x}Te has a more complex form:
Here, the LL index n runs over positive integers n=1,2, …. for the states in the electron and lighthole bands (ξ=±1). For the zero energy, flat heavyhole band (ξ=0), n runs over all nonnegative integers, except 1: n=0, 2, 3…. The quantum number σ accounts for the Kramer’s degeneracy lifted by the magnetic field B=(0, 0, B). The corresponding splitting can be viewed as the Zeeman (spin) splitting of LLs: E_{ξ,n,↑}(p_{z})−E_{ξ,n,↓}(p_{z}). The nonparabolicity of the bands implies a strong dependence of this spinsplitting on p_{z}, B and on LL and band indices.
Temperatureinduced bandgap opening in narrow gap HgCdTe
Besides the linear behaviour of the absorption coefficient at zero magnetic field measured in both samples (see Supplementary Fig. 1 and Supplementary Note 2), the presence of pseudorelativistic 3D fermions with is established at 2 K in the sample A by like dependence of optical transitions and a spin splitting of LLs seen in Fig. 2a. The fitting of the two main lines based on equation (2) shows that they are related to the interband transitions between the heavyhole band remaining at zero energy (ξ=0) and the n=1 spinup and spindown LLs with ξ=1 (for details, see Supplementary Figs 2 and 3). The extracted bandgap value at 2 K equals =(5±2) meV. Magnetooptical results obtained at temperatures from 57 to 120 K are shown in Fig. 2b–d. The bandgap, visualized by intersect of the interband transitions with the energy axis (shown by white arrows), increases with temperature (see also Supplementary Fig. 4). In addition to interband transitions (Δξ=1), intraband LLs transitions (Δξ=0) are also observed and fitted with equation (2).
Temperaturedriven phase transition
Magnetoabsorption of the sample B at different temperatures is presented in Fig. 3, in a scale for the sake of clarity. It is seen that at low temperatures and low magnetic field values, the LLs transitions exhibit some discrepancies compared with a pure behaviour. Indeed, as shown in Fig. 1, the linear energy dispersion in conduction and valence bands arises in gapless samples only. However, even in the case of small negative (or positive) gap, the bands could be considered as parabolic in the vicinity of the Γ point. It corresponds to the small values of parameter , for nonzero rest mass values. At low magnetic fields, the band parabolicity results in a linear behaviour of the LLs transitions as a function of B. Therefore, only a precise behaviour down to the lowest applied magnetic fields implies a system with genuine massless particles. At temperatures below T_{C}, the deviation from a pure behaviour is well reproduced by the theory and gives absolute values of the rest mass approaching to zero when temperature increases. As seen in equation (2), linear extrapolation of optical transitions in the squareroot scale intersects the energy axis at , as represented by arrows in Fig. 3a,b. An accurate behaviour for all optical transitions is obtained as an evident proof of gap closing at 77 K (Fig. 3c, see also Supplementary Fig. 5). Above the critical temperature, the difference in energies of inter and intraband transitions in low magnetic fields becomes visible, as it is for the sample A, meaning that a positive gap between the Γ_{6} and Γ_{8} bands opens. This allows us claiming that at T_{C}=77 K, a temperaturedriven topological phase transition with pseudorelativistic massless Kane fermions occurs. This fact is highlighted by the change of a sign of particle rest mass seen in Fig. 4a.
Universal velocity and rest mass description
The rest mass extracted from magnetooptical data and its dependence on temperature is compared with theoretical values using Supplementary equation (1)^{21} (in Supplementary Note 1). In the sample A, the rest mass is positive and increases in the whole range of temperatures, as it is shown in Fig. 4a. As discussed above, in the sample B the Kane fermion rest mass experiences a change of sign corresponding to the temperatureinduced semimetaltosemiconductor topological phase transition, which occurs at 77 K. Supplementary equation (1)^{21} (in Supplementary Note 1) describes very well the experimental rest mass curves for both samples and clearly reproduces the phase transition at 77 K in the sample B. The conic dispersion relation of the massless particles can be therefore realized for the specific range of crystal chemical composition and an according temperature—conditions that provide that the bulk bandgap is fully closed. Interestingly, the Kane fermion velocity is nearly constant over the whole range of temperatures for both samples with Cd contents of 0.155 and 0.175. The extracted value of ^{−1} is in a very good agreement with the theoretical value defined by which equals to for the wellaccepted value of E_{P}=2m_{0}P^{2}/ħ^{2}≈18.8 eV (ref. 22). Therefore, this universal value of allows for determination of the particle rest mass for bandgap values in the vicinity of the semimetaltosemiconductor phase transition induced by temperature, Cd content or other external parameter (for example, pressure). Figure 4c shows the variation of the experimental bandgap energy obtained in this work (full blue and red points) and from previous studies^{21,23,24} (open symbols), as a function of the rest mass, using and the universal value of .
Discussion
There are two points limiting the applicability of the simplified Kane model, considering the Γ_{6} and Γ_{8} band only, for actual HgCdTe crystals. The first one, already mentioned above, is related to the existence of other bands, considered as remote and not included in the model. The energy gap between the second and the lowest conduction bands in CdTe exceeds 4 eV, while the corresponding gap in HgTe is about 3 eV (ref. 25). Therefore, the cutoff energies for conduction bands in the simplified model should be lower than 3 eV. For the valence band, the cutoff energy is defined by the energy difference Δ≈1 eV between the splitoff Γ_{7} band and the heavyhole band. The second limitation is attributed to the flat heavyhole band, characterized by an infinite effective mass in the model. To ignore the parabolic terms in the electron dispersion of the heavyhole band, one has to consider sufficiently low energies E, such that the relativistic mass of the fermions should be significantly lower than the heavyhole mass m_{hh}. Assuming m_{hh}≈0.5m_{0}, where m_{0} is the free electron mass, we arrive at a cutoff energy of ∼3 eV for the flat band approximation, which exceeds Δ.
By using temperature as a finetuning external parameter we measured the bandgap energy of HgCdTe bulk crystals with wellchosen chemical composition in the vicinity of the semimetaltosemiconductor phase transition. We clearly observed and accurately measured increasing of the bandgap with temperature in sample A. We also observed genuine massless Kane fermions at the critical temperature of 77 K in sample B. We used the simplified Kane model to determine the pseudorelativistic Kane fermion parameters and as a function of temperature and Cd content. We observed a change of sign of accounting for the temperaturedriven topological phase transition. Our results also reveal universal velocity in HgCdTe crystals allowing for the determination of the Kane fermion rest mass from all experimental results in the literature obtained in the vicinity of the phase transition.
Methods
Experimental details
We performed magnetooptical studies on two [013]oriented Hg_{1−x}Cd_{x}Te layers, with different Cd concentrations, x=0.17 and 0.155. Both films were sufficiently thick (≈3.2 μm) to be considered as 3D materials and thin enough to be transparent in the farinfrared spectral range. The samples were grown by molecular beam epitaxy on semiinsulating GaAs substrates with relaxed CdTe buffers^{26}. We used a special ultrahigh vacuum multichamber molecular beam epitaxy set, which allows for the growth of very highquality HgCdTe crystals monitored by in situ reflection highenergy electron diffraction and single wavelength ultrafast ellipsometry (0.5 nm).
The magnetooptical transmission measurements were carried out by using a Fourier transform spectrometer coupled to a 16 T superconducting coil. The radiation of a Globar lamp is guided to a sample using oversized waveguides (light pipes). The intensity of the transmitted light is measured by a silicon bolometer. Both the magnet and the bolometer require cryogenic temperatures; therefore, most of reported up to today experiments were conducted at 4.2 K or lower temperatures. In this work, to perform a temperature tuning of the band structure, the standard magnetooptical configuration required important modifications. The bolometer was placed in a vacuum chamber separated from the sample chamber. To provide a wide spectral range for experiments, an indiumsealed cold diamond window ensures the optical coupling between the transmitted light and the bolometer. An additional superconducting coil around the bolometer compensates the spread field of the main coil, keeping the bolometer at zero magnetic field. This additional compensating superconducting coil also provides an additional screening of the bolometer. A Lambda plate coil—placed below the main magnet allows to obtain superfluid helium around the bolometer and keep the main coil at 4 K. Therefore, this modified experimental setup allows to keep the coils in their superconducting state, the bolometer at its optimal temperature and to tune the sample chamber temperature in the 2–150 K range.
The magnetooptical spectra were measured in the Faraday configuration up to 16 T, with a spectral resolution of 0.5 meV. All the spectra were normalized by the sample transmission response at B=0 T.
Simplified Kane model
Relativistic fermions are usually described by the Dirac equation:
where p_{i} (i=x, y, z) are the components of momentum operator, m and c are the rest mass and velocity of light, respectively. The matrices α_{i} and β define the symmetry properties of the particles and have the form
in which σ_{i} are the Pauli matrices and I is a 2 × 2 unit matrix. As it is clearly seen from equation (3), if the rest mass of particles equals zero, their dispersion is described by twofold degenerate cone in energymomentum space.
Current physics has proven the existence of several bulk condensedmatter materials, which are fairly well described by the above equation. At the same time, there are also other systems with relativisticlike charge carriers; nevertheless, they are described by different Hamiltonians. For Kane fermions, the corresponding Hamiltonian formally resembles the one for genuine 3D Dirac particles. However, we see that it has a form of a 6 × 6 matrix, which describes qualitatively a different system:
where , , , and where U_{c}, J_{x}, J_{y}, J_{z} are 3 × 3 matrices described as follows:
Here we deliberately present lowenergy Hamiltonian, which describes the Kane fermions in a form similar to the Dirac equation, defining the rest mass and velocity of the Kane fermions. The matrices J_{x}, J_{y}, J_{z} arising in equation (5) do not satisfy the algebra of angular momentum 1; therefore, the Hamiltonian does not reduce to any wellknown case of relativistic particles. However, the Kane fermions, with the Hamiltonian described by equation (5), share a number of properties with other relativistic particles.
Data availability
The data that support the findings of this study are available from the corresponding authors on request.
Additional information
How to cite this article: Teppe, F. et al. Temperaturedriven massless Kane fermions in HgCdTe crystals. Nat. Commun. 7:12576 doi: 10.1038/ncomms12576 (2016).
References
 1.
Novoselov, K. S. et al. Twodimensional gas of massless Dirac fermions in graphene. Nature 438, 197–200 (2005).
 2.
Hasan, M. & Kane, C. L. Colloquium: topological insulators. Rev. Mod. Phys. 82, 3045–3067 (2010).
 3.
Qi, X. L. & Zhang, S.C. Topological insulators and superconductors. Rev. Mod. Phys. 83, 1057–1110 (2011).
 4.
Dziawa, P. et al. Topological crystalline states in Pb_{1−x}Sn_{x}Se. Nat. Mater. 11, 1023–1027 (2012).
 5.
Liu, Z. K. et al. A stable threedimensional topological Dirac semimetal Cd_{3}As_{2}. Nat. Mater. 13, 677–681 (2014).
 6.
Lv, B. Q. et al. Observation of Weyl nodes in TaAs. Nat. Phys. 11, 724–727 (2015).
 7.
Yang, L. X. et al. Weyl semimetal phase in the noncentrosymmetric compound TaAs. Nat. Phys. 11, 728–732 (2015).
 8.
Orlita, M. et al. Observation of threedimensional massless Kane fermions in a zincblende crystal. Nat. Phys. 10, 233–238 (2014).
 9.
Malcolm, J. D. & Nicol, E. J. Magnetooptics of massless Kane fermions: role of the flat band and unusual Berry phase. Phys. Rev. B 92, 035118 (2015).
 10.
Martyniuk, M., Dell, J. W. & Faraone, L. in Mercury Cadmium Telluride: Growth, Properties and Applications (eds P. Capper & J. W. Garland) 153–204John Wiley & Sons, Chichester (2010).
 11.
Kane, E. O. in Narrow Gap Semiconductors Physics and Applications: Proceedings of the International Summer School Held in Nimes, France 3–15 September 1979 (ed. W. Zawadzki). Lecture Notes Phys. 133, 13–31 (1980).
 12.
Kane, E. O. Band structure of narrow gap semiconductors. Narrow Gap Semicond. Phys. Appl. 133, 13–31 (1980).
 13.
Bernevig, B. A., Hughes, T. L. & Zhang, S. C. Quantum spin Hall effect and topological phase transition in HgTe quantum wells. Science 314, 1757–1761 (2006).
 14.
Jiang, Z. et al. Infrared spectroscopy of Landau levels of graphene. Phys. Rev. Lett. 98, 197403 (2007).
 15.
Henriksen, E. A. et al. Interactioninduced shift of the cyclotron resonance of graphene using infrared spectroscopy. Phys. Rev. Lett. 104, 067404 (2010).
 16.
Sadowski, M. L., Martinez, G., Potemski, M., Berger, C. & de Heer, W. A. Landau level spectroscopy of ultrathin graphite layers. Phys. Rev. Lett. 97, 266405 (2006).
 17.
Chen, Z.G. et al. Observation of an intrinsic bandgap and Landau level renormalization in graphene/boronnitride heterostructures. Nat. Commun. 5, 4461 (2014).
 18.
Ludwig, J. et al. Cyclotron resonance of singlevalley Dirac fermions in nearly gapless HgTe quantum wells. Phys. Rev. B 89, 241406 (R) (2014).
 19.
Orlita, M. et al. Magnetooptics of massive Dirac fermions in bulk Bi_{2}Se_{3}. Phys. Rev. Lett. 114, 186401 (2015).
 20.
Chen, R. Y. et al. Magnetoinfrared spectroscopy of Landau levels and Zeeman splitting of threedimensional massless Dirac fermions in ZrTe_{5}. Phys. Rev. Lett. 115, 176404 (2015).
 21.
Laurenti, J. P. et al. Temperature dependence of the fundamental absorption edge of mercury cadmium telluride. J. Appl. Phys. 67, 6454–6460 (1990).
 22.
Novik, E. G. et al. Band structure of semimagnetic Hg_{1−y}Mn_{y}Te quantum wells. Phys. Rev. B 72, 035321 (2005).
 23.
Rigaux, C. Interband magnetooptics in narrow gap semiconductors. Narrow Gap Semicond. Phys. Appl. 133, 110–124 (1980).
 24.
Dornhaus, R. & Nimtz, G. in The Properties and Applications of the Hg_{1x}Cd_{x}Te Alloy System vol. 98, ed. Gerhard Höhler119–281Springer Tracts in Modern Physics (1983).
 25.
Chadov, S. et al. Tunable multifunctional topological insulators in ternary Heusler compounds. Nat. Mater. 9, 541–545 (2010).
 26.
Dvoretsky, S. et al. Growth of HgTe quantum wells for IR to THz detectors. J. Electron. Mater. 39, 918–923 (2010).
 27.
Sheregii, E. M., Cebulski, J., Marcelli, A. & Piccinini, M. Temperature dependence discontinuity of the phonon mode frequencies caused by a zerogap state in HgCdTe alloys. Phys. Rev. Lett. 102, 045504 (2009).
 28.
Polit, J. et al. Additional phonon modes related to intrinsic defects in CdHgTe. Phys. Stat. Solid. C 6, 2012–2015 (2009).
 29.
Rumyantsev, V. V. et al. Spectra and kinetics of THz photoconductivity in narrowgap Hg_{1–x}Cd_{x}Te (x< 0.2) epitaxial films. Semicond. Sci. Technol. 28, 125007 (2013).
 30.
Guldner, Y., Rigaux, C., Mycielski, A. & Couder, Y. Magnetooptical investigation of Hg_{1−x}Cd_{x}Te. Phys. Stat. Sol. (b) 81, 615–627 (1977).
Acknowledgements
We acknowledge M. Dyakonov, W. Zawadzki and A. Raymond for helpful discussions. This work was supported by the CNRS through LIA TeraMIR project, by the LanguedocRoussillon region and the MIPS department of Montpellier University via the Terahertz platform, by European cooperation through the COST action MP1204, and the Era.NetRus Plus project ‘Terasens’. F.T. and S.S.K. acknowledge the support from the Physics Department (INP) of CNRS for postdoc prolongation program. This work was also supported by the Russian Academy of Sciences, the nonprofit Dynasty foundation, the Russian Foundation for Basic Research (Grants 140231588, 155216017, 150208274 and 160200672), by Russian Ministry of Education and Science (grant numbers MК6830.2015.2 and HIII1214.2014.2) and by NTSIL. J.L., S.M., Z.J. and D.S. acknowledge the support from the U.S. Department of Energy (grant number DEFG0207ER46451) for infrared spectroscopy measurements at 4.2 K that were performed at the National High Magnetic Field Laboratory, which is supported by National Science Foundation (NSF) Cooperative Agreement Number DMR1157490 and the State of Florida.
Author information
Affiliations
Laboratoire Charles Coulomb, UMR CNRS 5221, University of Montpellier, Montpellier 34095, France
 F. Teppe
 , M. Marcinkiewicz
 , S. S. Krishtopenko
 , S. Ruffenach
 , C. Consejo
 , A. M. Kadykov
 , W. Desrat
 , D. But
 & W. Knap
Institute for Physics of Microstructures, Russian Academy of Sciences, Nizhny, 603950 GSP105 Novgorod, Russia
 S. S. Krishtopenko
 , A. M. Kadykov
 , S. V. Morozov
 & V.I. Gavrilenko
Institute of High Pressure Institute Physics, Polish Academy of Sciences, 01447 Warsaw, Poland
 W. Knap
National High Magnetic Field Laboratory, Tallahassee, Florida 32310, USA
 J. Ludwig
 , S. Moon
 & D. Smirnov
Department of Physics, Florida State University, Tallahassee, Florida 32306, USA
 J. Ludwig
 & S. Moon
Laboratoire National des Champs Magnétiques Intenses, CNRSUJFUPSINSA, 38042 Grenoble, France
 M. Orlita
Faculty of Mathematics and Physics, Charles University, Ke Karlovu 5, 121 16 Prague 2, Czech Republic
 M. Orlita
School of Physics, Georgia Institute of Technology, Atlanta, Georgia 30332, USA
 Z. Jiang
Lobachevsky State University of Nizhny Novgorod, Nizhny, 603950 Novgorod, Russia
 S. V. Morozov
 & V.I. Gavrilenko
Institute of Semiconductor Physics, Siberian Branch, Russian Academy of Sciences, pr. Akademika Lavrent’eva 13, 630090 Novosibirsk, Russia
 N. N. Mikhailov
 & S. A. Dvoretskii
Novosibirsk State University, 630090 Novosibirsk, Russia
 N. N. Mikhailov
 & S. A. Dvoretskii
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Contributions
The experiment was proposed by F.T. The theory was formulated by S.S.K. The samples were grown by N.N.M. and S.A.D. The samples were characterized by M.O., A.M.K., W.D., D.B., S.V.M., V.I.G., D.S., J.L., S.M. and Z.J. The temperaturedependent magnetooptical experimental setup was built by C.C., S.R., F.T. and W.K. Magnetooptical experiments were performed by M.M., S.R., F.T., D.S. and C.C. All coauthors discussed the data. F.T., D.S. and W.K. wrote the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to F. Teppe.
Supplementary information
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Supplementary Information
Supplementary Figures 15, Supplementary Notes 12 and Supplementary References
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