Weyl Fermion magneto-electrodynamics and ultralow field quantum limit in TaAs

Infrared spectroscopy in high magnetic fields reveals the lowest quantum limit in a Weyl semimetal.

Abstract

Topological semimetals are predicted to exhibit unconventional electrodynamics, but a central experimental challenge is singling out the contributions from the topological bands. TaAs is the prototypical example, where 24 Weyl points and 8 trivial Fermi surfaces make the interpretation of any experiment in terms of band topology ambiguous. We report magneto-infrared reflection spectroscopy measurements on TaAs. We observed sharp inter-Landau level transitions from a single pocket of Weyl Fermions in magnetic fields as low as 0.4 tesla. We determine the W2 Weyl point to be 8.3 meV below the Fermi energy, corresponding to a quantum limit—the field required to reach the lowest LL—of 0.8 tesla—unprecedentedly low for Weyl Fermions. LL spectroscopy allows us to isolate these Weyl Fermions from all other carriers in TaAs, and our result provides a way for directly exploring the more exotic quantum phenomena in Weyl semimetals, such as the chiral anomaly.

INTRODUCTION

Weyl semimetals are a novel class of quantum materials featuring electronic band structures with chiral Weyl Fermions (1–3) and arc like surface states (4, 5). Weyl Fermions arise at points in the Brillouin zone where conduction and valence bands have protected crossings that arise from strong spin-orbit coupling. When time reversal and inversion symmetry are preserved, these points are fourfold-degenerate and are commonly known as Dirac points. When one of these symmetries is broken, however, the band crossings are double-degenerate—these are the Weyl points. Weyl points come in pairs, with each point having a well-defined chirality or “handedness.” The electronic band structure near the Weyl points can be described using an effective model given by the Weyl equation, first introduced for chiral, massless (linearly-dispersing) fermions in high energy physics (6). The electrodynamics of Weyl Fermions can be highly nontrivial, with phenomena that have no counterpart in regular metals such as the chiral anomaly. Because their prediction and subsequent discovery by Angle-resolved photoemission spectroscopy (ARPES) experiments (4, 5), Weyl semimetals have attracted a great deal of attention, both for their unusual electrodynamics and as a platform for discovering new quantum phases of mater such as monopole superconductivity (7).

However, experimental characterizations of the electrodynamics of Weyl Fermions have been significantly hampered by the complicated band structures that are found in real materials, in contrast to the ideal Weyl fermions described by the Weyl equation. In addition to “Weyl pockets”—the segments of Fermi surface that surround the Weyl points when the chemical potential is not at the band-crossing point—most Weyl systems also contain trivial (non-Weyl) Fermi surfaces. Many Weyl materials have their Weyl points far from the chemical potential, making any connection between the observed behavior and the underlying band topology dubious at best. Finding a material with the simplest band structure or using a technique that can isolate the response of a single carrier type is therefore essential for understanding the electrodynamic properties of Weyl Fermions.

The tantalum and niobium monopnictides (TaAs, TaP, NbAs, and NbP) are one of the simplest and most widely explored families of Weyl semimetals. Among these, TaAs has the simplest low energy electronic band structure (8). In the Nb-based compounds, there are trivial pockets that are very close in momentum space to the Weyl nodes and even merged into the Fermi surface of the Weyl pocket, which makes it almost impossible to selectively probe a particular Weyl node without contributions from the trivial pocket (8, 9). In addition, the Weyl points in the Nb-based compounds are separated by saddle points that are only about 20 meV apart in energy, whereas this separation is around 100 meV in the Ta-based compounds (9, 10). This ensures that an effective two-band model captures the essential low energy physics in the Ta-based compounds (11, 12). Last, the Fermi surfaces enclosing the Weyl nodes of TaAs are much smaller than they are in TaP (9), making TaAs a great model system for probing the electrodynamics of Weyl Fermions.

Band structure calculations and ARPES measurements indicate that there are two sets of Weyl points in TaAs, labeled W1 and W2 in Fig. 1A. The pairs of nodes with opposite chirality (four W1 and eight W2 pairs) are distributed near the boundaries of the first Brillouin zone and are oriented perpendicular to the tetragonal axis (4, 9). TaAs has three distinct sections of Fermi surface, distributed around the dashed circle—a nodal line in the limit that spin-orbit coupling is zero—in Fig. 1A. The pockets that enclose the W1 Weyl points are highly anisotropic in their dispersion, with a smaller Fermi velocity along the crystal c axis. The pockets that enclose the W2 Weyl points are relatively isotropic in comparison. In addition to the Weyl Fermi surfaces, there are hole pockets that do not enclose any Weyl points: These are denoted as H1 (8, 9).

Fig. 1. Measurement scheme and inter-LL transitions in TaAs.

(A) Fermi surface of TaAs featuring Weyl pockets W1 and W2 and a trivial hole pocket H1—each distributed around the nodal line, represented by the dashed circle, which would be present with zero spin-orbit coupling [reprinted with permission from (21), copyright 2016 by the American Physical Society]. There are four such nodal lines and accompanying pockets arranged at the edges of the Brillouin zone in TaAs. (B) TaAs crystal with the flat surface in the ab plane. The schematic indicates the measurement geometry: The magnetic field is applied in the ab plane at an angle θ from the a axis. Reflected infrared light is collected in the Voigt configuration. (C) Schematic band structure for a pair of Weyl points with chirality χ = ±1 in a magnetic field. LLs labeled by index N are formed in the plane perpendicular to B field, while the momentum parallel to the magnetic field, k_//B, is still a good quantum number. The zeroth LLs at both Weyl points disperse as linear, one-dimensional (1D) bands. Inter-LL transitions obey optical selection rules Δ|N| = ±1. (D) 2D color plot of the infrared reflectivity in a magnetic field, normalized by the reflectivity at zero field (taken at θ = 45°). Sharp peaks that evolve with magnetic field are labeled by the proposed LL index of initial and final states. Because of the diverging density of states (DOS) at the band edge for each of the N > 0 LLs, peaks in (D) are dominated by inter-LL transitions at k_//B = ±k_w where the Weyl points are located.

Magneto-infrared spectroscopy has played an important role in characterizing topological phases of matter (13). In contrast to magneto-transport measurements, where the DC conductivity contains contributions from all Fermi surfaces superimposed on one another, infrared spectroscopy measurements can separate the responses of different Fermi surface into different frequency ranges. Previous efforts on Weyl semimetals, however, observed inter-LL transitions only in relatively high magnetic fields (> 5 T) and at high energies (> 40 meV), leaving the electrodynamics of Weyl Fermions in the immediate vicinity of the Weyl nodes unexplored. At the same time, the Faraday configuration (with magnetic field applied perpendicular to direction of Weyl point separation) used in previous measurements on TaAs mixes signals from the two different types of Weyl Fermions (14–17). Thus, an unambiguous identification of the low-energy electrodynamics from a single type of Weyl Fermion has not been reported.

RESULTS

We have used magneto-infrared reflection spectroscopy in the Voigt configuration, with the magnetic field in the ab plane (see Methods and Fig. 1B), to examine the low energy dynamics of Weyl Fermions around the W2 Weyl point of TaAs (Fig. 1A). The Voigt configuration, combined with sharp LLs due to high sample quality, allows us to observe inter-LL transitions from only the W2 Weyl pocket and at a much lower field strength and energy range than previously reported for any other Weyl semimetal.

We applied the magnetic field in the ab plane so that the Fermi surface around the W1 Weyl points has a larger cross-sectional area perpendicular to the magnetic field direction than if the field was applied along the c axis. This results in a smaller cyclotron energy for quasiparticles on the W1 Fermi surface, making their contribution to the optical conductivity a featureless continuum across our entire field range. In contrast, the relatively isotropic W2 Fermi surface has a much smaller Fermi surface area perpendicular to the magnetic field. This results in a larger cyclotron energy (about one order of magnitude larger than that of W1) and well-separated peaks in the optical conductivity spectrum from inter-LL transitions.

Because the polished surface of our TaAs crystals is parallel to the ab plane, this choice of magnetic field direction corresponds to the Voigt configuration of reflection spectroscopy, as shown in Fig. 1B. Under an applied magnetic field, electron motion perpendicular to the field direction is quantized into LLs with index N, as shown in Fig. 1C. These LLs evolve into a series of one-dimensional (1D) bands dispersing along k_//B, which is still a good quantum number in a magnetic field. In this case, van Hove singularities (vHSs) in the density of states (DOS) are located at k_//B = 0, and interband optical transitions from/to these vHSs are expected to dominate the optical conductivity spectrum. In the Voigt configuration, these optical transitions obey selection rules Δ|N| = ±1 for light polarization perpendicular to B and Δ|N| = 0 for polarization parallel to B (18).

Figure 1D shows the experimental reflection spectrum as a function of magnetic field. At zero magnetic field, the reflection spectrum of TaAs is expected to be smooth due to the absence of LLs and their accompanying vHSs. We focus on the magnetic field–induced features, which are revealed by normalizing the spectrum at finite field by that at zero field. At a fixed magnetic field as low as 0.4 T, we observed oscillations in the normalized spectrum that indicate the emergence of quantized LLs. These oscillations gradually evolve into several branches as we increase the magnetic field. These features correspond to inter-LL transitions, as expected from the schematic in Fig. 1C. The branch at the lowest energy is very broad in energy: We assign it to the transition 0➔ 1 and −1➔ 0. The breadth in energy of this transition is due to the lack of a vHS in the joint DOS (jDOS) for this transition: (i) the zeroth LL lacks a DOS vHS due to its linear dispersion; (ii) transitions between the almost parallel part of the N = 0 and N = ±1 LL bands at large k_//B should have a vHS in jDOS, but they are forbidden by Pauli blocking (i.e., all states are either unoccupied or occupied in the region where N = 0 and N = ±1 are parallel). All other branches of magnetic field–induced features are sharp in energy due to vHSs (at the same k_//B) for both the initial and final states, corresponding to the inter-LL transitions. For now, we assume that these transitions are from the W2 Weyl Fermi surfaces; we later confirm this assumption by examining the scaling with field and the extracted Fermi velocity. We tentatively assign the dispersing features to pairs of LL indices, each corresponding to Δ|N| = ±1, as shown in Fig. 1D.

Next, we examine the scaling relation of the inter-LL transition energies as a function of magnetic field. Figure 2A shows the normalized reflectance on a log-log plot. The four major branches of features can be fit with a scaling of E ∝ B^{0.62 ± 0.05}. This is close to the E ∝ B^0.5 scaling expected for the perfect linear dispersion of ideal Weyl cones and distinct from the E ∝ B scaling expected for trivial, parabolic bands. This rules out the trivial hole pocket H1 as the source of the LL transitions.

Fig. 2. Scaling of inter-LL transition energies with magnetic field.

(A) 2D color plot of the normalized reflectance spectrum in the range of B = 0.3 to 7 T. Both axes are plotted on a log scale. The color scale is the same as in Fig. 1D. The dominant inter-LL transitions can be described phenomenologically by a scaling of E ~ B^{0.62 ± 0.05}, as indicated by dashed lines. The deviation of the scaling from B^0.5—expected for a perfectly linearly-dispersing bands near the Weyl points—is expected due to the curvature of the band near the saddle point that connects the two Weyl points (see the Supplementary Materials for details). (B) Comparison between the experimental inter-LL transition energies and those calculated from a model Hamiltonian that incorporates the saddle point (see the Supplementary Materials for details). The four branches of features in (A) and Fig. 1D agree well with calculated dispersions plotted in black, red, green, and blue, from low to high energy. These transitions are attributed light polarization perpendicular to B.

To further clarify the origins of the inter-LL transitions and to understand the precise origin of the ∝ B^{0.62 ± 0.05} scaling, we use a two-band Hamiltonian that describes the electronic structure of Weyl points separated along k_//B (11, 12)

$$H\left(\mathit{k}\right)=a(k_w^2-k^2){\mathrm{\sigma }}_z+\mathrm{\hslash }{v}_F(k_x{\mathrm{\sigma }}_x+k_y{\mathrm{\sigma }}_y)$$ (1)

where σ_ι is the ith Pauli matrix and v_F is the Fermi velocity. The two Weyl nodes sit at (0, 0, ±k_w). This minimal Hamiltonian gives a global description of a pair of Weyl nodes with opposite chirality and preserves all of their topological properties (12). This Hamiltonian can be further reduced to

$$H(\mathit{k})=-a{k}^2{\mathrm{\sigma }}_z+\mathrm{\hslash }{v}_F\mathit{k}·\mathrm{\sigma }$$ (2)

near each Weyl point by redefining k_z ± k_w → k_z, where a characterizes the height of the saddle point between the two Weyl nodes (see fig. S1). Equation 2 can be quantized analytically in the presence of a magnetic field, and, from the resultant LL energies, we reproduce dispersions of the experimentally observed transitions, as shown in Fig. 2B. The four major transitions traced by dashed lines in Figs. 2A agreed well with the calculated Δ|N| = ±1 transitions. They are excited by light polarization perpendicular to the B field. Note that the correction to the B^0.5 scaling expected for perfectly linear bands emerges naturally in this model by incorporating curvature along the k_w direction. At higher energy—above 100 meV—the dispersion deviates from B^0.62 scaling but the model that incorporates that the saddle point continues to describe the inter-LL transitions up to the highest measured magnetic field of 17.5 T (see fig. S5 for additional data). In addition, there are branches of weaker features in Figs. 1D and 2A whose energy dispersions are close to those calculated for Δ|N| = 0 transitions. It is likely that these branches of features are excited by light polarization parallel to the B field, as our light source is largely unpolarized (see section S5 for further discussion) (18).

The Fermi velocity we extract by fitting the LL transition spectra is 2.2 ± 0.1 × 10⁵ m/s, which agrees well with the Fermi velocity at the W2 Weyl point extracted from previous quantum oscillation measurements and theoretical predictions (8, 9, 19, 20). The extracted Fermi velocity is one order of magnitude larger than what is expected for W1 Weyl point in this field orientation (9). It is also more than a factor of two smaller than the Fermi velocity measured via quantum oscillations for the trivial hole pocket (21), which, in addition, should have LLs that disperse linearly or near linearly in field. We therefore conclude that all major features observed in our experiment correspond to inter-LL transitions from the W2 Weyl pockets and not from the W1 Weyl pockets or the trivial H1 pockets. We find that the curvature parameter in Eq. 2, a = 0.5 eV nm², provides the best fit to the data.

In addition to characterizing the band dispersion around the Weyl points, inter-LL transitions provide a direct way to measure the distance of the Fermi energy, E_F, from the Weyl points. The Fermi surface areas for the W1 and H2 pockets in TaAs are consistent across multiple groups (19–22), suggesting that E_F is determined by band alignment within the crystal and that impurity doping plays a minimal role in setting the chemical potential (17). The position of E_F directly determines the threshold magnetic field at which the quantum limit is reached—when all LL bands other than N = 0 are either filled or empty, leaving only the two N = 0 LL bands with opposite chirality partially filled. Figure 3A illustrates how E_F can be measured by the inter-LL transitions. We assume that the Weyl cone is electron-like so that the Fermi level is above the Weyl point, consistent with previous work (8, 9, 19, 20), although our results are insensitive to this assignment. At low magnetic fields, inter-LL transitions below Fermi level at k_//B = ±k_w are forbidden due to Pauli blocking—there can be no transitions from an occupied state to another occupied state. The corresponding branch of transitions will therefore not show up in the reflectance spectrum at low field. As B increases to a critical value, the Nth LL band edge is raised to the Fermi level, unblocking the −(N − 1)➔N transition. The corresponding branch of inter-LL transition features will then emerge in the reflectance spectrum as the field is increased beyond the critical value. We measure the threshold fields and energies of the inter-LL transitions to extract the distance from the Weyl node to E_F, as shown in Fig. 3A. Here, we assume the band around the Weyl point has a linear dispersion for simplicity. Nonlinear corrections to the dispersion used in Fig. 2C are smaller than the uncertainty and thus negligible (see section S3).

Fig. 3. Extraction of Fermi energy and quantum limit of the Fermi surface at the W2 Weyl points.

(A) Illustration of the scheme for measuring the distance between the Weyl points and the Fermi energy, E_F. When B is increased so that the band edge of the Nth LL band is aligned with E_F, the inter-LL band transition −(N − 1)➔ N is no longer blocked. The corresponding branch appears in the reflectance spectrum at an energy $E=E_{\mathrm{F}}(1+\frac{\sqrt{N-1}}{\sqrt{N}})$. E₁ is the energy of the first LL band edge measured from the Weyl point at zero energy. The quantum limit is reached when E_F = E₁. (B) 2D color plot of the normalized reflectance spectrum in the range of 0.1 to 2 T and 5 to 30 meV. The black triangle, red diamond, green dot, and blue square indicate the threshold fields of the four main branches. Their corresponding energies and magnetic fields are listed to the right of the plot.

Figure 3B shows a 2D plot of inter-LL transitions in the range of B = 0.1 to 2 T. These data were taken in much finer steps than in Fig. 1D to reveal the details of the onset of the inter-LL transitions. Each major branch of features emerges beyond a threshold field and energy. Using the energies of these threshold points, we estimate the distance between E_F and the Weyl points as 7.6, 7.7, 8.6, and 9.2 meV (from the −1➔2, −2➔3, −3➔4, and − 4➔5 branches, respectively). We therefore concluded that E_F is 8.3 ± 0.9 meV above the W2 Weyl points in TaAs. We further determine the magnetic field at which the quantum limit is reached to be B_QL = B_N*$\sqrt{N}$ (by definition, the quantum limit is reached when the first LL band edge emerges from below E_F). Using the threshold magnetic field B_N obtained from Fig. 3B, we extract the values of B_QL as 0.99, 0.75, 0.74, and 0.74 T, respectively. Thus, we conclude that the quantum limit is B_QL = 0.8 ± 0.1 T for Fermi surface around the W2 Weyl points.

A quantum limit of 0.8 T is significantly lower than has previously been reported for any other Weyl semimetal (21–24). This includes prior studies of TaAs that compare quantum oscillations with band structure calculations, which suggested that the quantum limit of the W2 Fermi surface is between 5 and 8 T, depending on the field orientation (21, 22). Our measurements suggest that previous identifications of the W2 pocket are incorrect. This is likely due to the difficulty in uniquely assigning calculated quantum oscillation frequencies to branches in the measured oscillation spectrum—a task made particularly difficult in TaAs because both the W1 and W2 Weyl pockets have nearly the same cross-sectional area when the magnetic field is applied along the c axis.

To confirm that the other Fermi surfaces—the electron pockets centered around the W1 Weyl points and the hole pockets H1—have the same Fermi surface volume in our samples as reported previously, we measured quantum oscillations in the same sample used to perform the magneto-infrared optical measurements. We use pulse-echo ultrasound to measure quantum oscillations in the sound velocity. For field along the c axis, we see a dominant oscillation frequency of approximately 7.5 T, as reported previously [identified as W1 in (21) and W2 in (22)—the same Fermi surface but with reversed nomenclature]. With the field along the a axis, we find a dominant oscillation frequency of approximately 1.4 T. Both the mass and quantum oscillation frequency of this 1.4-T pocket are consistent with the trivial hole pocket identified in (see section S7 for details) (21). There is a peak in the Fourier transform of the quantum oscillations near 0.8 T that may correspond to the W2 pocket, but the frequency is so low that it is difficult to distinguish from the background. This highlights the difficulty in using quantum oscillations to identify Weyl fermions: Extremely low-frequency oscillations are lost in the background, and the damping factor due to scattering makes them even more difficult to observe before they reach their quantum limit.

Having established the main features of the magneto-electrodynamics of the Weyl Fermions at the W2 Weyl points, we now describe several experimental observations that allow for more accurate descriptions of the Fermi surface at W2. Figure 4A compares the inter-LL transition energies at three different in-plane angles θ over the same range of magnetic field. The redshift of the −1➔2 and −2➔1 branch of transitions shows a 20% relative change in energy as the field is rotated from θ = 45° to θ = 0°. This shift indicates anisotropy in the ab plane of momentum space for the W2 pockets. We propose an anisotropic shape for the W2 pockets as shown in Fig. 4B, consistent with the fourfold rotation and mirror reflection crystal symmetries of TaAs for this sample geometry. When the magnetic field is oriented 45° from the a or b axis, the cross section perpendicular to B is smaller than when the field is pointing along the a or b axis. This explains the angle dependence of inter-LL transition energies in Fig. 4A. While twofold symmetry in the ab plane is allowed for the W2 pockets based on their position in the Brillouin zone, twofold anisotropy would result in a qualitatively different θ dependence: Any twofold anisotropy must be below our experimental resolution (see fig. S2).

Fig. 4. Characterization of the anisotropy and fine features of the W2 Weyl Fermi surface.

(A) 2D color plots of the normalized reflectivity in the range of 5 to 6 T for three different angles: θ = 0°, 22°, and 45°. The color scale is shown in (C) but shared by (A), (C), and (D). The −1➔2 and −2➔1 branches redshift as the field is rotated from θ = 45° to θ = 0°, showing a relative change of 20%. (B) Possible shape of W2 Weyl pockets in the ab plane of the momentum space. W2 Weyl pockets lie in the k_a-k_b plane at a constant k_c = ±k_c^w2. Each pocket must have smaller (bigger) cross section along the 45° (0°) direction to explain the angle dependence of inter-LL transition energies. Because of the fourfold rotation symmetry and mirror reflection symmetries of the crystal lattice in the ab plane, the square-shaped W2 pockets is the only possible shape to explain the data in (A) (a lower, twofold symmetric pocket is allowed by symmetry but would produce features not seen in the data—any twofold distortion must be below our resolution). (C) Fine splitting within the −1➔2 and −2➔1 branch and the −2➔3 and −3➔2 branch at θ = 45°, indicating possible electron-hole asymmetry. (D) A linecut of Fig. 3B at B = 1.1 T. Three fine peaks, separated by ~1.5 meV, can be resolved. This observation implies a linewidth of inter-LL transitions on the order of 1.5 meV and small inhomogeneous broadening.

In addition to the anisotropy of the W2 Fermi surfaces, we observe fine features within the same branch of the inter-LL transitions, as shown in Fig. 4C. The peaks are split with an energy difference of approximately 8%, possibly indicating the breakdown of electron-hole symmetry and thus breaking the degeneracy between the −(N − 1)➔N and −N➔(N − 1) transitions.

Last, to quantify the crystal quality, we provide an estimate of the scattering rate of the Weyl Fermions in the W2 pockets. As shown in Fig. 4D, three dispersions of the inter-LL transition peaks can be resolved in the 2D color plot. By cutting a line at B = 1.1 T, we obtain an average peak separation of approximately 1.5 meV. Using the Rayleigh criteria, we conclude that the inhomogeneous broadening of inter-LL transition is less than 3 meV, corresponding to a scattering rate of 4.5 ps⁻¹ and a mean free path of 50 nm. This agrees well with the scattering rate measured via quantum oscillations in our samples grown previously (19). In addition, a high electron mobility (μ >30,000 cm²/V ∙ s) is extracted from the μ · B ≈ 1 criteria for the emergence of the Landau level transitions at less than 0.3 T.

DISCUSSION

We observed clear inter-LL transitions from the Fermi surface surrounding the W2 Weyl points of TaAs by using high-quality TaAs crystals and the Voigt configuration for magneto-infrared reflection spectroscopy. The observed scaling laws of the transition energies confirm an electronic dispersion that is characteristic of Weyl fermions, and we extract the curvature parameter that leads to small deviations from linear dispersion due to the small separation between the two Weyl points. Unexpectedly, we find that the magnetic field where the quantum limit is reached for this pocket is only 0.8 T—an order of magnitude smaller than previously reported (21–24). To the best of our knowledge, this is the lowest quantum limit field reported for any Weyl semimetal to date. This low quantum limit, and correspondingly low Fermi energy, makes TaAs favorable for further investigations of Weyl fermions. For example, one could incorporate a DC electric field in the ab plane into our measurement scheme using thin, fabricated TaAs devices or films. This would pump charge from one Weyl point to its neighbor of opposite chirality, raising the chemical potential of one point with respect to the other and splitting the single onset at the quantum limit into two. Such charge pumping is known as the chiral anomaly of Weyl Fermions (18, 25–28). Previous measurements of this effect relied on DC transport, which suffered from ambiguity due to other possible trivial effects (29–31). Our experiment suggests a more direct, spectroscopic measurement of this effect by directly probing the change in the chemical potential at each Weyl node induced by charge pumping. In addition, the distinct chirality and unique spin textures surrounding each Weyl point give rise to a new degree of freedom that is analogous to the valley degree of freedom in semiconductors. This has been studied through various techniques including photocurrent (32) and spin-resolved ARPES (33). By introducing a magnetic field in a manner similar to what we have done here, the chiral LL states with energy separation in the terahertz range may offer a new scheme for optoelectronic and spintronic devices. Last, we suggest that the energy-space separation offered by the LL spectroscopy that we use here is ideal for investigating the Weyl fermi surfaces of other materials where the fermiology is undetermined and likely complex, such as Mn₃Sn and Co₂MnGa.

METHODS

Sample growth and orientation

Millimeter-sized single crystals of TaAs were grown by means of an iodine-vapor transport technique with 0.05 g/cm³ I₂. First, polycrystalline TaAs was prepared by heating stoichiometric amounts of Ta and As in an evacuated silica ampoule at 973 K for 3 days. Subsequently, the powder was loaded in a horizontal tube furnace in which the temperature of the hot zone was kept at 1123 K and that of the cold zone was ~1023 K. The composition and structure of the TaAs single crystals was verified by Laue diffraction and energy-dispersive x-ray spectroscopy. No I₂ doping was detected.

Crystals were approximately aligned by their morphological structure, and the alignment was refined to better than 1° using Laue diffraction. Flat, ab-plane surfaces (perpendicular to the tetragonal c axis) were polished using 1-μm diamond lapping film and finished with 30-nm lapping film.

Magneto-infrared reflectance measurements

Broadband magneto-infrared measurements were performed using a Bruker 80v Fourier transform infrared spectrometer at liquid helium temperature with a superconducting magnet up to 17.5 T. The unpolarized broadband light from a globar was delivered to the sample through evacuated light pipes and focused on the sample in Voigt geometry. The sample was sitting at the field center in a helium exchange gas environment. The reflected light was collected and delivered to a Si bolometer placed away from the magnetic field center.

Supplementary Materials

This PDF file includes:

Sections S1 to S8

Figs. S1 to S8

References