Momentum-space signatures of Berry flux monopoles in the Weyl semimetal TaAs

Since the early days of Dirac flux quantization, magnetic monopoles have been sought after as a potential corollary of quantized electric charge. As opposed to magnetic monopoles embedded into the theory of electromagnetism, Weyl semimetals (WSM) exhibit Berry flux monopoles in reciprocal parameter space. As a function of crystal momentum, such monopoles locate at the crossing point of spin-polarized bands forming the Weyl cone. Here, we report momentum-resolved spectroscopic signatures of Berry flux monopoles in TaAs as a paradigmatic WSM. We carried out angle-resolved photoelectron spectroscopy at bulk-sensitive soft X-ray energies (SX-ARPES) combined with photoelectron spin detection and circular dichroism. The experiments reveal large spin- and orbital-angular-momentum (SAM and OAM) polarizations of the Weyl-fermion states, resulting from the broken crystalline inversion symmetry in TaAs. Supported by first-principles calculations, our measurements image signatures of a topologically non-trivial winding of the OAM at the Weyl nodes and unveil a chirality-dependent SAM of the Weyl bands. Our results provide directly bulk-sensitive spectroscopic support for the non-trivial band topology in the WSM TaAs, promising to have profound implications for the study of quantum-geometric effects in solids. Weyl semimetals exhibit Berry flux monopoles in momentum-space, but direct experimental evidence has remained elusive. Here, the authors reveal topologically non-trivial winding of the orbital-angular-momentum at the Weyl nodes and a chirality-dependent spin-angular-momentum of the Weyl bands, as a direct signature of the Berry flux monopoles in TaAs.

T opological semimetals have become a fruitful platform for the discovery of quasiparticles that behave as massless relativistic fermions predicted in high-energy particle physics [1][2][3][4][5][6] . A prominent example are Weyl fermions, which are realized at topologically protected crossing points between spin-polarized electronic bands in the bulk band structure of noncentrosymmetric or ferromagnetic semimetals 1,2,[7][8][9][10][11] . Near a Weyl node the momentum-resolved two-band Hamiltonian takes the form H ∝ ±σ ⋅ k, giving rise to the linear energy-momentum dispersion relation of a massless quasiparticle 4 . The topological structure of the Weyl node, however, is not encoded in the energy spectrum, but rather manifests in the momentum-dependence of the eigenstates, i.e., the electronic wave functions. The pseudospin σ and the Berry curvature Ω wind around the Weyl node, forming a Berry flux monopole in three-dimensional (3D) momentum space 12,13 . The nontrivial winding of σ stabilizes the Weyl node by a topological invariant, a nonzero Chern number of C = ±1 (ref. 4 ).
Until today, angle-resolved photoelectron spectroscopy (ARPES) experiments have confirmed a number of materials as Weyl semimetals (WSM), based on a comparison of the measured bulk band structure to band calculations and the observation of surface Fermi arcs 1,9,10,14,15 . Manifestations of the nontrivial topology have also been found, accordingly, in magnetotransport experiments 16 , by scanning tunneling microscopy 17 , and via optically induced photocurrents 18 . The winding of the electronic wave functions in momentum space, however, which characterizes the immediate effect of a Berry flux monopole and thus the topology of the WSM, has so far remained elusive.
While the pseudospin σ for a Dirac-Hamiltonian universally shows nontrivial winding, the underlying microscopic degrees of freedom may vary from one system to another 19 . In two dimensions, examples include the sublattice degree of freedom for graphene and the spin-angular momentum (SAM) for the surface states in topological insulators (TI). Accordingly, the nontrivial Berry-phase properties have been addressed by quasiparticle interference STM imaging and dichroic ARPES in graphene 20,21 and by spin-resolved ARPES in TI 22 . Likewise in 3D WSM, one may expect the relevant degrees of freedom to depend on the considered material system. While previous theories have suggested orbital-sensitive dichroic effects in momentum-resolved spectroscopies, as a probe of topological characteristics in topological semimetals [23][24][25] , such approaches have previously not reached application to experimental data.
In the present work, we find that the orbital-angular momentum (OAM) L plays a crucial role in the Weyl physics of the paradigmatic WSM TaAs and, like the pseudospin σ, displays a topologically nontrivial winding at the Weyl points. Our experiments are based on soft X-ray (SX) ARPES, which allows for the systematic measurement of bulk band dispersions by virtue of an increased probing depth and excitation into photoelectron final states, with well-defined momentum along k z perpendicular to the surface 26 , when compared to surface-sensitive ARPES experiments at VUV photon energies. SX-ARPES has been the key method to probe chiral-fermion dispersions in topological semimetals 1,2,5,[27][28][29] , but its combination with spin resolution (SR) and circular dichroism (CD) is challenging and not widely explored 30 . On the other hand, at lower excitation energies SR is routinely used to detect the SAM of electronic states 22 and CD has been introduced as a way to address the OAM [31][32][33][34][35] . We performed SX-ARPES measurements combined with SR and CD to probe the SAM and OAM in the bulk electronic structure of TaAs.

Results
Bulk band structure of TaAs. TaAs crystallizes in the noncentrosymmetric space group I4 1 md, as shown in Fig. 1a. According to the results of first-principles calculations, its bulk band structure features 12 pairs of Weyl points in the Brillouin zone, which divide into two inequivalent sets, W 1 and W 2 (refs. 7,8 ). Here, we focus on the W 2 points which are located in k x -k y planes at k z ¼ ± 0:59 2π c , with the length c along z denoting the conventional unit cell. In agreement with earlier works 1,2 , our SX-ARPES data in Fig. 1 predominantly reflect the bulk bands of TaAs, allowing us to address the bulk band structure through variation of the photon energy. The experimental dispersions along the ΓΣ and ZS high-symmetry lines compare well with the calculated bands ( Fig. 1c-d). We further performed hν-dependent measurements to trace the band dispersion along k z , for which we likewise achieve agreement with theory ( Fig. 1e and Supplementary Note 1). Based on this, we determine a photon energy of approximately hν = 590 eV that allows us to reach a final-state Fig. 1 Bulk electronic structure of TaAs. a Bulk crystal structure of TaAs with space group I4 1 md. b Experimental geometry of the angle-resolved photoemission spectroscopy (ARPES) experiment using circularly polarized soft X-ray radiation. c, d ARPES data sets along the ΓΣ and ZS high-symmetry directions of the bulk Brillouin zone. e ARPES data set along k z at k x = −0.53 Å −1 , corresponding to the calculated k x position of the W 2 Weyl nodes (cut Z in f). In c-e, the red lines represent the calculated band dispersion. f Bulk Brillouin zone structure in the k x -k z plane. W 2 Weyl nodes at k z ¼ 23 :41 2π c are addressed at a photon energy of approximately hν = 590 eV (cf. Figs. 2 and 3). The star marks the (k x ,k z ) position of the data set in Fig. 2a.
momentum corresponding to the W 2 Weyl points within experimental uncertainty (Fig. 1e, f).
Orbital and spin-angular momentum of the bulk states. The formation of Weyl nodes in TaAs relies on the coexistence of inversion-symmetry breaking (ISB) and spin-orbit coupling (SOC) 7,8 , which induces a spin splitting into nondegenerate bands. The results of our first-principles calculations in Fig. 2a, b show this splitting for the bulk valence and conduction bands, which split up into branches v + and v − , as well as c + and c − , respectively. Note that the crossing points between the upper valence band v + and the lower conduction band c − define the Weyl nodes in TaAs (see below). Going beyond the band dispersion, we explore the impact of ISB and SOC on the electronic wave functions. According to our calculations, the key consequence of ISB is the formation of a sizable OAM L in the Bloch wave functions ( Fig. 2a and Supplementary Fig. 3). The spin-split branches in the valence and conduction band carry parallel OAM, while the SAM is antiparallel (Fig. 2a, b). This indicates a scenario for the bulk states in TaAs, where the energy scale associated with ISB dominates over the one of SOC 32,33,36 (see also Supplementary Fig. 4). Moreover, our calculations show that v ± and c ± carry opposite OAM, indicating that the Weyl nodes are crossing points between bands of opposite OAM polarization.
To confirm the formation of OAM experimentally, we measured the CD signal, i.e., the difference in photoemission intensity for excitation with right and left circularly polarized light, which has been shown to be approximately proportional to the projection of L on the light propagation direction k p (refs. 31,32 ). The grazing light incidence in the xz-plane of our experimental geometry (Fig. 1b), thus implies that the measurements predominantly reflect the L x component of the OAM. Note that the relation between CD and OAM, derived in refs. 31,32 , relies on the free-electron final-state approximation, which can be expected to hold particularly well at the high excitation energies used in the present experiment. Indeed, a comparison of the measured CD to the L x -projected band structure shows a remarkable agreement over wide regions in momentum space, as seen in Figs. 2a and 3a, b. The detailed match between experimental data and theory proves that the measured CD indeed closely reflects the momentum-resolved local OAM of the bulk states in TaAs. As expected theoretically 31,32 , the OAM of the initial state is thus the most important source of CD under the present experimental conditions as opposed to mere geometric or final-state effects. Particularly the latter can become relevant at lower excitation energies, where the final state is not wellapproximated in the free-electron picture 37,38 .
While OAM is induced by ISB already in the absence of SOC, the presence of Weyl nodes requires a SOC-induced formation of spin polarization 7,8 . An experimental proof of spin-polarized bulk states in TaAs and related transition-metal monopnictides has remained elusive up to now. Our spin-resolved SX-ARPES measurements directly verify the predicted SAM of the bands v ± . They confirm an opposite S x for v + and v − (Fig. 2b-e), while our CD-ARPES data prove a parallel alignment of L x , in line with our calculations (Fig. 2a). Moreover, the spin-resolved data confirm an opposite sign of S x at +k y and −k y . Overall, our experiments establish sizable OAM and SAM polarizations of the bands forming the Weyl nodes in TaAs.
Circular dichroism and OAM near the Weyl nodes. To explore the momentum-dependence of the OAM in more detail, we consider momentum distributions of the measured CD and the calculated L x for the band v ± in an equi-k z plane of the W 2 nodes (Fig. 3a, b). Besides the good agreement of experiment and theory, it is evident from the data that the Weyl-node pair near k x = −0.5 Å −1 , marked in Fig. 3b, is located at a distinctive position within the OAM texture. A quantitative comparison of the CD and the calculated OAM along k x paths through the two Weyl nodes of opposite chirality is shown in Fig. 3c. The experiment reveals sign changes of L x close to the Weyl nodes and an opposite overall sign of L x for the two nodes, consistent with the To examine the OAM and CD of the Weyl cone, we focus on the band dispersion along k x across a W 2 Weyl node in Fig. 4a-e. For the band v + , which forms the lower part of the Weyl cone, the two branches on the left and on the right side of the Weyl node are selectively probed by the circular light polarization: using right circularly polarized light (Fig. 4d), there is a high photoemission intensity for the left branch of v + , while the right branch is suppressed. Vice versa, for left circularly polarized light, we find the left branch to be suppressed, while the right branch is more strongly excited (Fig. 4e). Accordingly, the band v + , shows an inversion of OAM across the Weyl node (Fig. 4b). This behavior is supported by a quantitative analysis of the intensities, shown in Fig. 4c. These observations indicate an opposite OAM for the upward and downward dispersing branches of v + and thus an OAM sign change across the Weyl node, in agreement with our calculations. It is noteworthy that the magnitude of the CD in general does not reach 100%, as seen, e.g., from the analysis in Fig. 4c.
The fact that the Weyl node is located slightly below the Fermi level further allows us to estimate the relative OAM orientation of the lower and the upper part of the Weyl cone. In Fig. 4h, we consider energy distribution curves (EDC) at a wave vector k x close to the Weyl node. A three-peak structure is observed in the EDC and attributed to the bands v − , v + , and c − . The CD for the bands v + and c − is opposite confirming the opposite OAM of these bands predicted by our calculations (Fig. 4b-e). Note that for left circularly polarized light the intensity of the band v + drops toward the Fermi energy, which, in combination with finite linewidth broadening, gives rise to some deviations between the CD signal and calculated OAM in Fig. 4b (see also Supplementary Figs. 10-12 for a more detailed discussion). In particular, unlike for the band v + , our present data does not allow us to discern a CD reversal of the band c − across the Weyl point close to the Fermi level.
Our measurements and calculations in Fig. 4 directly image characteristic modulations of the Bloch wave functions near the W 2 Weyl nodes. Further evidence for momentum-dependent changes also of the L y component near the W 2 nodes is presented in Supplementary Fig. 9. It is important to note that the observed sign reversal of L x across the Weyl node is not enforced by any symmetry. Rather, it reflects a true band-structure effect that characterizes the Weyl-fermion wave functions, namely the crossing of two bands carrying opposite OAM (Fig. 4b-e). This situation is different from the surface states in TI 22,31 or related examples 39,40 , where a sign reversal across the nodal point is strictly imposed by time-reversal or crystalline symmetries. From an experimental point of view, this makes the presently observed sign reversal of L x more forceful, as it is a band-structure-specific and not a symmetry-imposed texture change.
Topological winding of OAM and Berry curvature. Our results reveal a close correspondence between measured CD and calculated OAM. In this work, the OAM is computed in the local limit by projecting the Bloch wave function onto atom-centered spherical harmonics, i.e., we consider the quantum-mechanical expectation value of the atomic L angular momentum operator. This approach offers a viewpoint complementary to the OAM given by the modern theory of polarization 41 . The fact that the CD rather corresponds to the local OAM 31,32 could be related to the local nature of the photoemission process itself 42 .
The formation of OAM, which we observe here, provides direct evidence for the influence of ISB on the bulk Bloch states and, thus, suggests that these states also carry finite Berry curvature Ω, which likewise originates from ISB. In Fig. 4f, we consider momentum distributions of CD and L x for the band v + , revealing a characteristic sign change along the contour around the Weyl nodes. The calculated momentum texture of the Ω x -component of the Berry curvature qualitatively resembles the characteristics of the OAM and the measured CD (Fig. 4f), suggesting that these quantities reflect the topologically nontrivial winding of the wave functions near the Weyl nodes 21,34,35,43 . Indeed, our calculations show explicitly that for TaAs the nontrivial topology of the Berry flux monopoles is encoded in the momentum-dependence of the OAM, while the SAM shows topologically trivial behavior. The topological nature of the field configuration is determined by the c , corresponding to the W 2 Weyl nodes. The data sets were obtained by integrating over an energy range from 0 eV to −1.2 eV, the width of the bands v ± (cf. Fig. 2a). The calculated positions of the W 2 Weyl nodes are indicated in b. The CD-ARPES data were acquired at hν = 590 eV. c CD signal normalized to the total photoemission intensity and L x component of the OAM along k x cuts through Weyl nodes of opposite chirality. Sign changes are observed near the Weyl nodes.
Pontryagin index calculated on a sphere surrounding the Weyl point where n is the unit vector of the field and the integral is taken over the 2D manifold covering the sphere. S is proportional to the Berry phase in momentum space accumulated by electrons encircling the Weyl point. In our calculations, the Pontryagin index of the vector fields of Berry curvature and OAM is S = 1 (Fig. 4g), while the SAM has S = 0 ( Supplementary Fig. 8).
Analogously to the Berry curvature, the Pontryagin index of the OAM is nonvanishing only if the sphere surrounds a Weyl node, and changes sign when the other Weyl node of the pair is considered. The Berry flux monopoles in TaAs thus derive from the orbital degrees of freedom of the electronic wave functions, and their topology manifests in a nontrivial texture winding of the OAM. We indeed theoretically verified that in the WSM TaP 44 and LaAlGe 45 the Pontryagin index of the OAM vector field winds around the type-I Weyl nodes. Interestingly, LaAlGe hosts two type-I and one type-II Weyl dispersions 46 . Our analysis brings further evidence of a nontrivial winding of OAM only at type-I Weyl cones (see also Supplementary Note 5), raising intriguing questions about the underlying conditions of spectroscopic manifestations of Berry flux monopoles. Preliminary investigations suggest that non-symmorphic symmetries and a large atomic-angular momentum (d orbitals involved in the low-energy description) may play a decisive role. Irrespectively, our work shows that the OAM can constitute-though not universally-an experimentally accessible quantity that reflects the nontrivial band topology in a WSM.
Energy hierarchy of ISB and SOC. For two-dimensional systems, the formation of OAM due to ISB has been shown to be the microscopic origin of SOC-induced spin splittings 36,47 . The present experiments establish a first instance where OAMcarrying bands are observed in a 3D bulk system. Our observations of SAM and OAM in TaAs indicate that an OAM-based origin of the spin splitting also applies to bulk systems with ISB and, as such, underlies the WSM state at the microscopic level. Specifically, the relative alignments of OAM and SAM in the bands v ± , determined from our CD-ARPES and spin-resolved data (cf. Fig. 2), imply an energy hierarchy of the bulk band structure in which ISB dominates over SOC 32,33 . In this case, the electronic states can be classified in terms of their OAM, as SOC does not significantly mix states of opposite OAM polarization. The reversal of L x , that we observe at the Weyl node, thus indicates an orbital-symmetry inversion accompanying the crossing of valence and conduction bands in TaAs. This supports an earlier theory predicting that the Weyl-semimetal state in TaAs originates from an inversion between bands of disparate orbital symmetries 7 .

Discussion
Previous SX-ARPES experiments succeeded in measuring the bulk band dispersion in WSM and other topological semimetals 1,2,5,6,28,29,48 . The present experiment for TaAs goes beyond the dispersion and probes the spin-orbital-components of the wave functions, which encode the topological properties. Our measurements unveil a characteristic reversal in the OAM texture of the bulk Weyl-fermion states at momenta consistent with the termination points of the surface Fermi arcs in TaAs 1,9,48 . Together, this constitutes a remarkably explicit spectroscopic manifestation of bulk-boundary correspondence in a WSM. In this regard, our results push forward the use of circularly polarized light as a probe of Weyl-fermion chirality to the momentum-resolved domain 18 .
Our results open a pathway to probe SAM and OAM textures in the bulk band structures of recently discovered magnetic WSM with broken time-reversal symmetry 10,11 , and of other topological semimetals hosting chiral fermions of higher effective pseudospin and higher Chern numbers, and thus with topological properties distinct from Weyl fermions 5,6,28,29,49 . This may allow to address the topological features in these band structures. For example, DFT calculations indicate a topological winding of the SAM at the Weyl nodes in the magnetic WSM HgCr 2 Se 4 (ref. 50 ). More broadly, our results establish a possibility of probing the topological electronic properties of a condensed matter system directly from a bulk perspective without resorting to the corresponding boundary modes.

Methods
Experimental details. We carried out SX angle-resolved photoemission spectroscopy (SX-ARPES) experiments at the ASPHERE III endstation at the Variable Polarization XUV Beamline P04 of the PETRA III storage ring at DESY (Hamburg, Germany). SX photons with a high degree of circular polarization impinge on the sample surface under an angle of incidence of α ≈ 17°(cf. Fig. 2b). TaAs single crystals were cleaved in situ with a top-post at a temperature <100 K and a pressure better than 5 × 10 −9 mbar. ARPES data were were collected using a SCIENTA DA30-L analyzer at a sample temperature of~50 K and in ultra-high vacuum <3 × 10 −10 mbar. The angle and energy resolution of the ARPES measurements was ca. Δθ ≈ 0.1°and ΔE ≈ 50 meV. Spin-resolved ARPES was performed by use of a Mott detector (Scienta Omicron). The Au scattering target had an effective Sherman function of 0.1. The energy resolution was ca. ΔE ≈ 600 meV, while the angle resolution was Δθ ≈ 6°in k x direction. The CD-ARPES and spin-resolved ARPES data were obtained using the deflection mode of the spectrometer, so that the experimental geometry stays fixed during the data acquisition procedures.
The growth of single crystals was performed via chemical vapor transport reactions. Sealed silica ampoules with inner diameter of 14 mm and length of 10 cm were loaded with Ta foil and As chunks in a stoichiometric ratio so that the total mass of the reactants was 1.2 g. After adding 0.055 g I 2 as transport agent, the ampoules were sealed airtight under a vacuum of ≈10 −5 mTorr. Then they were loaded into a single zone tube furnace with a defined temperature gradient across the length of the tube. The angle of the crucibles against the horizontal was ≈20°. The temperature was increased from room temperature up to 640°C at 5 K h −1 , where it was held constant for 24 h and subsequently heated to 1000°C at a rate of 2.5 K h −1 . Crystal growth proceeded over the following 3 weeks in a temperature gradient of 1000°C: 950°C (ref. 51 ). After cooling radiatively to room temperature, TaAs single crystals with a volume up to 2 mm 3 were obtained. The crystal structure and stoichiometry were confirmed using single-crystal X-ray diffraction 52 and energy dispersive X-ray spectroscopy methods (Zeiss 1540 XB Crossbeam Scanning Electron Microscope).
Theoretical details. We consider in our theoretical study the noncentrosymmetric primitive unit cell of TaAs (space group I4 1 md) with a lattice constant of 6.355 Å. We employ state-of-the-art first-principles calculations based on the density functional theory as implemented in the Vienna ab initio simulation package (VASP) 53 , within the projector-augmented plane-wave (PAW) method 54,55 . The generalized gradient approximation as parametrized by the PBE-GGA functional for the exchange-correlation potential is used 56 by expanding the Kohn-Sham wave functions into plane waves up to an energy cutoff of 400 eV. We sample the Brillouin zone on an 8 × 8 × 8 regular mesh by including SOC selfconsistently 57 . For the calculation of the OAM, the Kohn-Sham wave functions were projected onto a Ta s, p, d-, and As s, p-type tesseral harmonics basis as implemented in the WANNIER90 suite 58 . The OAM expectation values were then obtained in the atom-centered approximation by rotating the tesseral harmonics basis into the eigenbasis of the OAM-operator, i.e., the spherical harmonics.

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