Article | Open

Strong interface-induced spin–orbit interaction in graphene on WS2

  • Nature Communications 6, Article number: 8339 (2015)
  • doi:10.1038/ncomms9339
  • Download Citation
Received:
Accepted:
Published online:

Abstract

Interfacial interactions allow the electronic properties of graphene to be modified, as recently demonstrated by the appearance of satellite Dirac cones in graphene on hexagonal boron nitride substrates. Ongoing research strives to explore interfacial interactions with other materials to engineer targeted electronic properties. Here we show that with a tungsten disulfide (WS2) substrate, the strength of the spin–orbit interaction (SOI) in graphene is very strongly enhanced. The induced SOI leads to a pronounced low-temperature weak anti-localization effect and to a spin-relaxation time two to three orders of magnitude smaller than in graphene on conventional substrates. To interpret our findings we have performed first-principle electronic structure calculations, which confirm that carriers in graphene on WS2 experience a strong SOI and allow us to extract a spin-dependent low-energy effective Hamiltonian. Our analysis shows that the use of WS2 substrates opens a possible new route to access topological states of matter in graphene-based systems.

Introduction

Because of the Dirac nature of its charge carriers and the presence of two valleys, graphene is a two-dimensional topological insulator1,2. Topological state characteristics have not been observed experimentally, because the strength of the spin–orbit interaction (SOI) intrinsically present in graphene is too weak3,4,5. Various strategies to amplify the SOI strength have been proposed theoretically6–8 or explored experimentally11. However, increasing the SOI strength in graphene without drastically affecting other basic aspects of its electronic structure, or the material quality, is proving extremely difficult11. Here we explore whether it is possible to induce strong SOI while preserving the quality of graphene, by exploiting interfacial interactions12,13,14 at an atomically sharp interface between graphene and a semiconducting WS2 crystalline substrate.

Many semiconducting transition metal dichalcogenides, such as WS2, are ideal substrates for graphene. Like hexagonal boron nitride (hBN)15, they are atomically flat and chemically inert, which is key to preserving high-quality transport properties (mobility values as high as μ50,000–60,000 cm2 V–1 s–1 have been recently reported for graphene on WS2) (ref. 16). Transition metal dichalcogenide crystals consist of a stack of monolayers having a hexagonal lattice that—like graphene—leads to the presence of two valleys in their electronic structure at the K and K′ point of the Brillouin zone17. The SOI in WS2 is extremely strong—several hundreds of millivolts in the valence bands and several tens of millivolts in the conduction band—and in monolayers it pins spin to valley18,19,20. The spins of states near the band edges point in one direction in one of the valleys and in the opposite direction in the other, a behaviour resembling the one expected theoretically in disorder-free graphene1,2. The ability of this substrate material to induce a strong SOI in graphene—as well as the nature of the induced SOI—is, therefore, an important topic that has attracted recent attention10.

Here we address these issues by combining a study of low-temperature quantum transport in graphene-on-WS2 devices with ab initio electronic structure calculations. Specifically, we perform systematic magnetotransport measurements to show that when transferred onto WS2 substrates graphene exhibits a pronounced and robust weak anti-localization (WAL) effect throughout the explored carrier density and temperature range, down to 250 mK. The detection of WAL provides a direct demonstration of the SOI enhancement in graphene due to the interfacial interactions with WS2 substrate. In the attempt to estimate quantitatively the magnitude of SOI enhancement, we show that the magnetotransport data can be fit to the theory of WAL for graphene in the presence of SOI, from which we determine the spin-relaxation time (τso). We find that the value of τso (2.5–5 ps) in graphene on WS2 is 100–1,000 times shorter than τso in pristine graphene on SiO2 or hBN. This very strong enhancement of SOI found experimentally is consistent with the result of our ab initio calculations, which indicate that hybridization with the WS2 substrate orbitals is responsible for the SOI induced in graphene, and estimate the SOI strength under the conditions of the experiments to be 5 meV. Finally, we show that the results of our calculations close to the K and K′ points can be mapped onto a long-wavelength effective Hamiltonian, which, depending on the values of the parameter, describes a topologically insulating state. We therefore conclude that the possibility of using interfacial interactions to induce a strong SOI in graphene while preserving the high quality of the material opens a new possible route to create and investigate a topological insulating state in graphene.

Results

High quality of graphene-on-WS2 device

We start by characterizing the basic transport properties of the graphene-on-WS2 devices used in our experiments. The devices are assembled in a multi–terminal Hall bar configuration, placed on a highly doped Si wafer that acts as a gate electrode and is coated with 280 nm SiO2 (see Fig. 1a for an optical microscope image, Fig. 1b,c for a schematic of the device structure and the Methods section for the details of the device fabrication). We have realized several such devices. Here we present representative data from one of them (similar data from another device can be found in the Supplementary Note 1 and Supplementary Fig. 1). Figure 1d shows that on ramping up the gate voltage from Vg=–40 V, the conductivity σ of graphene on WS2 decreases linearly until Vg8 V, after which it saturates. Saturation occurs because, for Vg>8 V, electrons are accumulated at the interface between the SiO2 and the WS2 crystal, screening the effect of the gate on the graphene layer on top (Fig. 1c, Supplementary Fig. 2 and Supplementary Note 2)21. (Because the mobility of charge carriers in WS2 is much smaller than in graphene22, carriers at the WS2/SiO2 interface give a negligible contribution to transport.) Sweeping the gate voltage down for Vg<8 V, on the contrary, results in an increase (Fig. 1b) of carrier (hole) density in graphene and the conductivity increases. In our devices, therefore, the position of the Fermi level can be gate shifted in the graphene valence band, but accumulation of electrons at the SiO2/WS2 interface prevents access to the conduction band. In the following we therefore study only hole transport through graphene. To illustrate this conclusion, and to start assessing the device quality, Fig. 1e–g shows that the half-integer quantum Hall effect characteristic of monolayer graphene23 is clearly observed for different values of Vg between –40 and 8 V. The longitudinal resistance measured in this Vg range, and plotted versus filling factor ν and magnetic field B (the inset of Fig. 1d), confirms this result. We estimate the carrier mobility from σ using the hole density n extracted from the (classical) Hall effect and by looking at the slope dσ/dVg, and obtain in both cases μ13,000 cm2 V–1 s–1 at T=4.2 K. Since no effort has yet been put into optimizing the fabrication process, these values confirm the very good quality of graphene-on-WS2 devices found in earlier work16.

Figure 1: Basic electrical transport properties of graphene-on-WS2 heterostructure at 250 mK.
Figure 1

(a) Optical microscope image of one of our devices, with multiple contacts in a Hall-bar geometry (scale bar, 10 μm). (b,c) Schematic cross-section of the device illustrating where charge is accumulated on varying Vg below and above 8 V (b and c, respectively). Owing to the presence of the n-doped WS2 substrate, charges are accumulated in graphene only for Vg lower than 8 V (the precise value slightly varies from sample to sample, depending on the doping level of the WS2 substrate.). (d) The conductivity (σ) of the device varies linearly with Vg, below 8 V, and saturates for larger Vg values (shadow area). The green dots mark the ranges of Vg (I: 0–5 V; II: −10 to −15 V; and III: −25 to −30 V) used to perform ensemble averages of the device magnetoconductance. (The inset shows Shubnikov-de Hass oscillation in the longitudinal resistance Rxx originating from the half-integer quantum-Hall effect characteristic of Dirac fermions, with the black regions corresponding to Rxx minima that occur at values of filling factor |ν|=|nh/eB|=4 × (N+1/2), with N being integer) (eg) Fully developed half-integer quantum-Hall effect with vanishing Rxx (black curve) and quantized Rxy (red curve) observed at different values of Vg=0, −11.5 and −28 V (from eg) within the region I, II and III (indicated in d).

Robust low-temperature WAL reveals strong SOI

To demonstrate the presence of SOI in our devices, we probe WAL, which usually manifests itself as a characteristic sharp magnetoconductance (MC) peak at B=0 T (refs 24, 25). In small, fully phase-coherent devices like ours, however, WAL is eclipsed by conductance fluctuations originating from the random interference of electron waves25,26. Indeed, in Fig. 2a, which shows the MC as a function of Vg and B, an enhancement in conductance at B=0 T is only faintly visible. No special feature at B=0 T can be detected by looking at a single MC curve measured at a fixed value of Vg (see, for example, the top curve shown in Fig. 2b measured at Vg=–25 V). The random conductance fluctuations, whose reproducibility is shown in Fig. 2c, can be suppressed through an ensemble averaging procedure in which MC traces measured at different Vg values are averaged25. The Vg spacing should be chosen to shift the Fermi level by Thouless energy of the system. It is expected that the root mean square amplitude of the fluctuations decreases as N−1/2 (N is number of uncorrelated MC traces used to calculate the average), eventually making the sharp conductance peak at B=0 T due to WAL visible, if the strength of SOI is sufficient. This is indeed what the experiments show (Fig. 2b,d,e).

Figure 2: Ensemble averaging of the MC at 250 mK.
Figure 2

(a) Colour-coded MC, ΔG(B), as a function of Vg, with the background conductance slowly varying in Vg subtracted. The large background conductance fluctuations originating from phase-coherent interference of electron waves are apparent, and nearly completely obscure the effect of WAL around B=0 T. (b) Evolution of the averaged MC on increasing the number N of uncorrelated MC traces used to calculate the average (N=1, 9 and 25; curves offset for clarity): the conductance peak at zero B associated to WAL becomes apparent for sufficiently large values of N. (c) Two MC traces measured at Vg=−25 V (red and black curves) demonstrating the excellent reproducibility of the conductance fluctuations. (d) After averaging over N different curves, the root mean square amplitude of the conductance fluctuations (δG) decreases proportionally to N−1/2 as expected for a proper ensemble-averaging process. (e) Zoomed-in view of the ensemble-averaged MC (for N=25), which clearly exhibits a sharp conductance peak at B=0 T.

We find that the WAL signal emerging from the ensemble average procedure is robust, and visible in the entire Vg range investigated. Its amplitude grows on lowering temperature T (Fig. 3a–c), and reaches 0.5 × e2/h at the largest negative Vg and T=250 mK (Fig. 3c), where e is electron charge and h is Planck’s constant. The phenomenon is not observed in graphene on conventional substrates such as SiO2 (refs 27, 28, 29) (or hBN30 or GaAs31), where at sub-Kelvin temperatures only weak localization is measured. This remark is important because in graphene WAL can occur also in the absence of SOI, due only to the Dirac nature of its charge carriers32,33,34. The WAL originating from the Dirac nature of electrons, however, is unambiguously different from what we observe on WS2 substrates: it is seen only for T10 K or higher, and has small amplitude, because its observation requires the phase coherence time τφ to be shorter than the intervalley scattering time τiv (ref. 28). The observation of the low-temperature MC shown in Fig. 3, therefore, represents a direct, unambiguous demonstration of the presence of SOI in graphene on a WS2 substrate.

Figure 3: Low-temperature WAL in graphene on WS2.
Figure 3

(ac) Ensemble-averaged MC curves (symbols) obtained from measurements performed in different ranges of Vg (I, II and III, respectively), at several different temperatures below 8 K. The square MC Δσ=σ(B≠0)–σ(B=0) clearly exhibits a peak at zero B in all Vg ranges, whose height decreases as temperature is increased from 250 mK to 8 K, the expected behaviour of WAL due to SOI. Solid lines show the best fits to equation (1) in the main text. (d) Carrier density dependence of the relevant characteristic times. The filled squares represent the elastic scattering time (τ) estimated from the conductivity of our device at zero B; the filled black (red) circles represent the spin relaxation time (τso) extracted from the analysis of WAL (non-local spin-Hall effect). For comparison, open up-triangles represent the values of intervalley scattering time (τiv) reported in the literature, and extracted from the analysis of weak-localization measured in device similar to ours on different substrates, such as SiO2 (black27 and red29), hBN (green30) and GaAs (blue31). Open circles represent τso obtained from spin-valve studies on pristine graphene on SiO2 (black37 and red38) and hBN (blue40). (e) Temperature dependence of the phase-coherence time (τφ) of electrons in graphene-on-WS2 extracted from the analysis of WAL performed in this work, for different gate-voltage ranges. The data clearly exhibit an increase in τφ with lowering temperature.

Very short spin relaxation time in graphene on WS2

To analyse the MC data quantitatively, we use the theory of WAL in graphene that considers the effect of all possible symmetry-allowed SOI terms in graphene, and predicts the following dependence of the low-temperature MC35:

Here is the rate of spin relaxation uniquely due to the SOI terms that break the z–z symmetry (z being the direction normal to the graphene plane), is the total spin relaxation rate due to all SOI terms present, =4DeB/ħ (D is the carrier diffusion constant) and F(x)=ln(x)(1/2+1/x) with the digamma function ψ(x). In fitting the data, we constrain all characteristic times to be independent of temperature, except for τφ, which increases on lowering T, as physically expected in the T range investigated. Equation (1) holds in the limit τφ>>τiv, which is the one physically relevant at low T, and reproduces the experimental results quantitatively (solid lines in Fig. 3a–c). The analysis allows us to obtain the relevant characteristic times τso, τasy and τφ, with a precision determined by the residual conductance fluctuations that are not perfectly removed by the ensemble averaging procedure. (These residual effects also cause σ to be non-perfectly symmetric on reversing B, because the conductivity is extracted from the conductance measured in a four-terminal configuration, which in fully phase coherent devices is in general not symmetric25.) We conservatively estimate the error on the characteristic times to be 50% in the worst case: although rather large as compared with what can be achieved in more established material systems, such an uncertainty is immaterial for all the considerations that will follow.

We find the spin-relaxation time to be τso2.5–5 ps depending on the value of Vg (see the black filled circles in Fig. 3d). Comparable values (within experimental uncertainties) have been obtained on the same devices from the analysis of measurements of non-local resistance generated by spin-Hall and inverse spin-Hall effect36 (see red circles in Fig. 3d, Supplementary Fig. 3 and Supplementary Note 3 for details). The latter technique was used recently in refs 9, 10 to probe SOI in hydrogenated graphene and graphene on WS2 in devices analogous to ours (see the Supplementary Note 4 for a comparison). The value of τasy is approximately three times larger than τso, consistent with its physical meaning; the phase coherence time τφ>>τso, as it must be since a large WAL signal is observed (see Fig. 3e; τφ decreases on increasing T, as expected). This internal consistency of the hierarchy of characteristic times extracted from fitting the data with equation (1) supports the validity of our analysis. We conclude that in graphene at a WS2 interface τso is 100–1,000 times shorter than τso for pristine graphene on SiO2 (refs 37, 38) or hBN39,40 (shown with open circles in Fig. 3d), and that such a large difference in strength must be due to substantially stronger SOI. In contrast to what has been reported in recent studies of graphene on WS2 (see ref. 10 and Supplementary Note 4), the larger strength persists throughout the entire gate voltage range investigated.

Determining the precise nature of the WS2-induced SOI is not straightforward. A customary way to extract information is to identify the spin-relaxation mechanism by looking at how τso depends on τ, the transport scattering time. Finding that τso increases with increasing τ points to the so-called Elliot–Yafet relaxation mechanism (spin relaxation mediated by scattering at impurities)41,42, whereas if τso decreases with increasing τ, the Dyakonov–Perel mechanism (typical of systems with a strong band SOI) may be invoked43. In graphene on SiO2 or hBN substrates, previous work has shown that neither scenario convincingly accounts for the observations8, which has led to both phenomenological approaches to describe the experimental data39, and to the theoretical proposal of new spin-relaxation mechanisms specific to graphene44. For graphene on WS2, despite the much larger strength of SOI, the interpretation of spin relaxation within the canonical schemes poses similar problems: τso decreases slightly on increasing τ (see Fig. 3d), ruling out Elliot–Yafet as a dominant relaxation mechanism, but the dependence is much weaker than the one predicted by Dyakonov and Perel, τso1, so that the data are not satisfactorily described by this mechanism either. One interesting observation, however, can be made by comparing the spin-relaxation time τso, with the intervalley scattering time τiv obtained from the analysis of weak localization in graphene on SiO2 (refs 27, 29), hBN30 and GaAs31. Literature values of τiv are shown with empty triangles in Fig. 3d: they are surprisingly narrowly distributed—they all fall within a factor of 2—if we consider that experiments have been performed by different groups and that different substrate materials are used. The values of τiv match well (again, within a factor of 2 or better) with τso obtained for graphene on WS2. This close correspondence between two a priori unrelated quantities is remarkable: it strongly suggests that the microscopic processes responsible for scattering between the two valleys are the same processes that cause spin flip in graphene on WS2.

Ab initio calculations of interface-induced SOI

To gain a better understanding of our experimental findings we have performed electronic structure calculations, to identify the dominant contributions to the WS2-induced SOI in graphene, and to verify that the large enhancement of the SOI strength we have discovered experimentally is indeed expected theoretically. Supercell electronic structure calculations were performed for a large number of crystal approximants to the incommensurate graphene-on-WS2 system. (See Supplementary Fig. 4 and Supplementary Note 5 for details.) The results demonstrate that hybridization between graphene and substrate orbitals adds SOI terms both to the graphene π-band Hamiltonian and to the π-band disorder Hamiltonian. For each approximant π-band states appear inside the WS2 gap Eg over a wavevector range of approximately Eg/ħvF surrounding both K and K′ Dirac points. Within this range π bands are accurately described by effective Hamiltonians of the form

where σ=(σx, σy, σz) is a Pauli matrix vector that acts on the sub lattice degree of freedom in graphene’s Dirac continuum model Hamiltonian H0, s=(sx, sy, sz) is a Pauli matrix vector that acts on spin and τz=±1 for K and K′ valleys (the corresponding dispersion relations are illustrated in Fig. 4). All three substrate-induced interaction terms are time-reversal invariant and absent by inversion symmetry in isolated graphene sheets. They arise from hybridization between carbon π orbitals and strongly spin–orbit split tungsten d orbitals in both valence and conduction bands of WS2. Unlike the Hamiltonians that describe graphene on hBN45, H in equation (2) is translationally invariant. This is so because the lattice constant difference between graphene and WS2 is much larger than for the case of graphene and hBN. As a consequence, the moiré pattern period is short, and superlattice effects couple states near the K and K′ points to states far away in momentum and energy that are outside the range accessible to transport experiments and describable in terms of modified π bands.

Figure 4: Low-energy band structure of graphene on WS2 near the K/K′ point.
Figure 4

(a) Comparison of the result of the ab initio calculations with the continuum model Hamiltonian discussed in the main text. The black dots represent the low-energy dispersion relation for graphene on WS2 as obtained from our density functional theory calculations, which can be fit with excellent precision with the dispersion relation obtained from equation (2) (red lines). (bd) Evolution of the low-energy dispersion relation of graphene as a function of SOI. (b) The usual Dirac cone for spin-degenerate charge carriers in isolated graphene close to the K/K′ point. (c,d) At an interface with a WS2 substrate, the dispersion relation is modified by the effect of the induced SOI. Ab initio calculations show that the low-energy Hamiltonian in equation (2) accurately describes the modifications to the band structure of graphene. Two SOI terms, with coupling constant λ and λR, are induced by interfacial interactions. Our calculations indicate that λ5 meV and λR1 meV. With these values the dispersion relation of electrons becomes the one shown in c that, at charge neutrality, corresponds to the band structure of an insulator (with non-trivial topological properties). The size of the gap is determined by the value of λR (as long as λ>>λR). Since the gap is likely small in our devices as compared with electrostatic potential fluctuations, λR can be neglected in a first approximation, in which case the dispersion relation becomes the one shown in d.

In our calculations, the importance of a spatially random intervalley contribution to SOI in real structures, which are not commensurate, is inferred from the observation that the numerical values of the substrate interaction parameters (Δ, λ and λR) depend on the supercell commensurability between graphene and WS2 triangular lattices (that is, the size of the approximant used in the calculation; see Supplementary Fig. 5). Physically, this dependence implies that spin-dependent terms that vary rapidly in space would be present even if each layer had a perfect, defect-free two-dimensional lattice. These terms can scatter graphene electrons between valleys via intermediate WS2 states. For this reason the continuum model of equation (2) should be supplemented by including random potential terms. (See the last paragraph of Supplementary Note 5 for a more complete explanation.) An estimate of the strength of these random potentials is given by the difference in the values of the parameters Δ, λ and λR obtained from calculations performed on approximants of different size (see Supplementary Fig. 5). This random spin-dependent substrate interaction provides a most plausible explanation for our finding that τso in graphene on WS2 is comparable to τiv.

As a quantitative estimate of the parameters Δ, λ and λR in equation (2) we take the values obtained from the calculations performed on the largest supercells that we have considered. The 9:7 ratio between the WS2 and graphene lattice constants in these supercells is very nearly in perfect agreement with experiment. We find that the interaction parameters implied by this commensurability are independent of rigid relative translations between graphene and the substrate, providing further support for the translational invariance of equation (2). They are however sensitive to the separation between graphene and substrate layers, which has not yet been accurately determined experimentally, but should be near 3 Å like for graphene on hBN46. For such a separation our calculations give Δ≈0 meV, λ≈5 meV and λR≈1 meV. The results illustrated in Supplementary Fig. 5 indicate that the value of λ is virtually the same for all approximants while larger relative fluctuations are found for Δ and λR, implying that it is these terms that dominate the random spatial potential responsible for intervalley scattering. Even though at this stage it is difficult to establish the precise role of the two different SOI contributions (the modification of the bands and the random potentials) to the shortening of the spin-relaxation time extracted from the experiments, our results show that the two larger SOI parameters exceed the scale of the SOI in isolated graphene sheets by two to three orders of magnitude3,4,5, and that sizable spin-dependent intervalley scattering is present. We therefore can conclude that the results of our calculations are consistent with the experimental observations, pointing unambiguously to a strong enhancement of SOI due to interfacial interactions in graphene on WS2.

Discussion

The general form of the Hamiltonian in equation (2), which yields a gap at charge neutrality because the Rashba term couples conduction and valence band states (compare Fig. 4c,d), deserves comment. It can be shown (see Supplementary Note 6) that when the Fermi energy lies in this gap and when λ is larger than Δ, the system becomes a topological insulator with gap larger by one to two orders of magnitude than that based on the intrinsic SOI in graphene originally proposed by Kane and Mele2. The result of our calculations for the largest supercell that we have considered (yielding Δ≈0 meV, λ≈5 meV and λR≈1 meV) should be therefore be viewed as a prediction that graphene on WS2 is a topological insulator. This is an exciting conclusion, because a SOI strength of a few meV brings the possibility to realize a topologically insulating state in graphene closer to what can be realistically achieved experimentally. Care should be taken, however, because the precise values of the parameters Δ, λ and λR may depend on the details of the calculations scheme employed. In particular, even if in our calculations the SOI strength was always found to have a few meV scale irrespective of the approximations made, it is difficult to conclude that Δ>λ in all cases (see Supplementary Note 7, where we discuss calculations in which we let the distance between graphene and WS2 relax). At this stage it seems that a reliable determination of the parameters in equation (2) with sufficient precision to conclusively determine whether graphene on WS2 is a topological insulator or not will require more experiments. Specifically, this may be possible through a careful investigation of the Shubnikov–de Haas oscillations in very-high-mobility devices, capable of detecting a splitting in their frequency and of investigating its precise gate voltage dependence.

The increase in spin–obit interaction strength induced in graphene by proximity with WS2 that we observe for all investigated values of gate voltage—and hence position of the Fermi energy—is a large effect, close to two orders of magnitude. It directly shows the relevance of interfacial interactions. Demonstrating the ability to combine the control given by these interactions with the high electronic quality inferred from the experiments is a key result: although clearly more optimization is needed, finding that a drastic increase in SOI strength can be achieved without compromising the electronic quality of graphene offers the possibility to improve the system quality even further. To this end, strategies already exist that largely benefit from the expertise developed for graphene and hBN, such as encapsulating graphene between two WS2 crystals16, using different device assembly techniques to avoid contact between graphene and unwanted materials during fabrication47, and optimizing the device-cleaning procedures48. As indicated by both our experimental results and their theoretical modelling, these developments open a possible route to access experimentally topological states49 in graphene, and will play an essential role in improving our understanding of the spin dynamics in this system.

Methods

Device fabrication

Thin WS2 flakes were exfoliated onto a highly doped silicon substrate acting as a gate covered by a SiO2, from high-quality single crystals of WS2 grown by chemical vapour transport method. These exfoliated WS2 flakes were annealed at 200 degrees for 3 h in an inert atmosphere, after which a specific WS2 flake with atomically flat and clean surface was identified through imaging with an atomic force microscope. Transfer of graphene onto the selected WS2 flake was achieved by means of (by now) common techniques15. Similarly to the case of other artificial stacks of atomically thin crystals, bubbles were found to form after transfer of graphene (visible as black points in Fig. 1a)30. To minimize the effect of these bubbles on the transport experiments, graphene was etched into a Hall-bar geometry, after electrodes consisting of a Ti/Au bilayer (10/70 nm) were defined by means of electron-beam lithography, electron-beam evaporation and lift-off. No post-annealing steps or other cleaning processes to further improve the device quality were performed on the devices discussed here. All transport measurements were performed in a He3 Heliox system with a base temperature of 250 mK. We investigated in full detail two monolayer devices showing identical results. The data presented in the main text are taken from one of the devices, which has a width of W=2.5 μm, and three pairs of Hall probes (the longest distance between different pairs of Hall probes in this device is 5.5 μm, see Supplementary Fig. 3b). The thickness of WS2 is about 26 nm. Data from the second monolayer device, virtually identical to the first one, are shown in the Supplementary Note 1.

Ab initio calculations

Fully relativistic density functional theory calculations were performed using the Vienna ab-initio Simulation Package with projector-augmented wave pseudopotentials under the generalized gradient approximation50,51. The graphene lattice constant was always kept at 2.46 Å. Ionic relaxations were performed for WS2 in 1 × 1 unit cells with lattice constants fixed to three different rational multiples (4/3, 5/4 and 9/7) of that of graphene. Supercells with different moiré periodicities were then constructed by repeating these unit cells correspondingly and by aligning the lattice vectors of WS2 with that of graphene without further ionic relaxation. The separation between graphene and WS2 was fixed to a number of different values ranging from 2.3 to 3.3 Å for each supercell. A Monkhorst-Pack k-point mesh52 of 6 × 6 × 1 was used for the 4 × 4 and 5 × 5 supercells (in terms of graphene lattice constant), and that of 3 × 3 × 1 was used for the 9 × 9 supercell. The plane wave energy cutoff was set to 400 eV in all calculations.

Additional information

How to cite this article: Wang, Z. et al. Strong interface-induced spin-orbit interaction in graphene on WS2. Nat. Commun. 6:8339 doi: 10.1038/ncomms9339 (2015).

References

  1. 1.

    & Z(2) topological order and the quantum spin Hall effect. Phys. Rev. Lett. 95, 146802 (2005).

  2. 2.

    & Quantum spin Hall effect in graphene. Phys. Rev. Lett. 95, 226801 (2005).

  3. 3.

    , & Spin-orbit coupling in curved graphene, fullerenes, nanotubes, and nanotube caps. Phys. Rev. B 74, 155426 (2006).

  4. 4.

    et al. Intrinsic and Rashba spin-orbit interactions in graphene sheets. Phys. Rev. B 74, 165310 (2006).

  5. 5.

    , & Tight-binding theory of the spin-orbit coupling in graphene. Phys. Rev. B 82, 245412 (2010).

  6. 6.

    & Impurity-induced spin-orbit coupling in graphene. Phys. Rev. Lett. 103, 026804 (2009).

  7. 7.

    , , , & Engineering a robust quantum spin hall state in graphene via adatom deposition. Phys. Rev. X 1, 021001 (2011).

  8. 8.

    , , & Graphene spintronics. Nat. Nanotechnol. 9, 794–807 (2014).

  9. 9.

    , , , & Colossal enhancement of spin-orbit coupling in weakly hydrogenated graphene. Nat. Phys. 9, 284–287 (2013).

  10. 10.

    et al. Spin-orbit proximity effect in graphene. Nat. Commun. 5, 4875 (2014).

  11. 11.

    et al. Spatial variation of a giant spin-orbit effect induces electron confinement in graphene on Pb islands. Nat. Phys. 11, 43–47 (2015).

  12. 12.

    et al. Hofstadter’s butterfly and the fractal quantum Hall effect in moire superlattices. Nature 497, 598–602 (2013).

  13. 13.

    et al. Massive Dirac fermions and Hofstadter butterfly in a van der Waals heterostructure. Science 340, 1427–1430 (2013).

  14. 14.

    et al. Cloning of Dirac fermions in graphene superlattices. Nature 497, 594–597 (2013).

  15. 15.

    et al. Boron nitride substrates for high-quality graphene electronics. Nat. Nanotechnol. 5, 722–726 (2010).

  16. 16.

    et al. Electronic properties of graphene encapsulated with different two-dimensional atomic crystals. Nano Lett. 14, 3270–3276 (2014).

  17. 17.

    , , , & Electronics and optoelectronics of two-dimensional transition metal dichalcogenides. Nat. Nanotechnol. 7, 699–712 (2012).

  18. 18.

    , & Giant spin-orbit-induced spin splitting in two-dimensional transition-metal dichalcogenide semiconductors. Phys. Rev. B 84, 153402 (2011).

  19. 19.

    , , , & Coupled spin and valley physics in monolayers of MoS2 and other group-VI dichalcogenides. Phys. Rev. Lett. 108, 196802 (2012).

  20. 20.

    , & Large spin splitting in the conduction band of transition metal dichalcogenide monolayers. Phys. Rev. B 88, 245436 (2013).

  21. 21.

    et al. Band offset and negative compressibility in graphene-MoS2 heterostructures. Nano Lett. 14, 2039–2045 (2014).

  22. 22.

    , , & Quantitative determination of the band gap of WS2 with ambipolar ionic liquid-gated transistors. Nano Lett. 12, 5218–5223 (2012).

  23. 23.

    , , , & The electronic properties of graphene. Rev. Mod. Phys. 81, 109–162 (2009).

  24. 24.

    , & Spin-orbit interaction and magnetoresistance in the two dimensional random system. Prog. Theor. Phys. 63, 707–710 (1980).

  25. 25.

    & in Solid State Physics eds Ehrenreich H., Turnbull D. Vol. 44, 1–228Academic (1991).

  26. 26.

    & Universal conductance fluctuations in metals. Phys. Rev. Lett. 55, 1622–1625 (1985).

  27. 27.

    , , & Weak localization in graphene flakes. Phys. Rev. Lett. 100, 056802 (2008).

  28. 28.

    , , & Transition between electron localization and antilocalization in graphene. Phys. Rev. Lett. 103, 226801 (2009).

  29. 29.

    & Rippled graphene in an in-plane magnetic field: effects of a random vector potential. Phys. Rev. Lett. 105, 146804 (2010).

  30. 30.

    et al. Random strain fluctuations as dominant disorder source for high-quality on-substrate graphene devices. Phys. Rev. X 4, 041019 (2014).

  31. 31.

    , , , & Magneto-transport properties of exfoliated graphene on GaAs. J. Appl. Phys. 110, 043712 (2011).

  32. 32.

    & Crossover from symplectic to orthogonal class in a two-dimensional honeycomb lattice. Phys. Rev. Lett. 89, 266603 (2002).

  33. 33.

    et al. Weak-localization magnetoresistance and valley symmetry in graphene. Phys. Rev. Lett. 97, 146805 (2006).

  34. 34.

    & Intervalley scattering, long-range disorder, and effective time-reversal symmetry breaking in graphene. Phys. Rev. Lett. 97, 196804 (2006).

  35. 35.

    & z-z symmetry of spin-orbit coupling and weak localization in graphene. Phys. Rev. Lett. 108, 166606 (2012).

  36. 36.

    , , & Nonlocal charge transport mediated by spin diffusion in the spin Hall effect regime. Phys. Rev. B 79, 035304 (2009).

  37. 37.

    , , , & Electronic spin transport and spin precession in single graphene layers at room temperature. Nature 448, 571–574 (2007).

  38. 38.

    & Spin relaxation in single-layer and bilayer graphene. Phys. Rev. Lett. 107, 047207 (2011).

  39. 39.

    , , & Long-distance spin transport in high-mobility graphene on hexagonal boron nitride. Phys. Rev. B 86, 161416 (2012).

  40. 40.

    et al. Controlling spin relaxation in hexagonal BN-encapsulated graphene with a transverse electric field. Phys. Rev. Lett. 113, 086602 (2014).

  41. 41.

    Theory of the effect of spin-orbit coupling on magnetic resonance in some semiconductors. Phys. Rev. 96, 266–279 (1954).

  42. 42.

    in Solid State Physics eds Seitz F., Turnbull D. Vol. 14, 1–98Academic (1963).

  43. 43.

    & Spin relaxation of conduction electrons in noncentrosymmetric semiconductors. Sov. Phys. Solid State 13, 3023–3026 (1972).

  44. 44.

    , , , & Pseudospin-driven spin relaxation mechanism in graphene. Nat. Phys. 10, 857–863 (2014).

  45. 45.

    , , & Ab initio theory of moire superlattice bands in layered two-dimensional materials. Phys. Rev. B 89, 205414 (2014).

  46. 46.

    et al. Cross-sectional imaging of individual layers and buried interfaces of graphene-based heterostructures and superlattices. Nat. Mater. 11, 764–767 (2012).

  47. 47.

    et al. One-dimensional electrical contact to a two-dimensional material. Science 342, 614–617 (2013).

  48. 48.

    et al. Mechanical cleaning of graphene. Appl. Phys. Lett. 100, 073110 (2012).

  49. 49.

    Topological Insulators in Contemporary Concepts of Condensed Matter Science Vol. 6 (eds Franz, M. & Molenkamp, L.) (Elsevier, 2013).

  50. 50.

    & Ab initio molecular dynamics for liquid metals. Phys. Rev. B 47, 558–561 (1993).

  51. 51.

    & Efficient iterative schemes for ab initio total-energy calculations using a plane-wave basis set. Phys. Rev. B 54, 11169–11186 (1996).

  52. 52.

    & Special points for Brillouin-zone integrations. Phys. Rev. B 13, 5188–5192 (1976).

Download references

Acknowledgements

We gratefully acknowledge technical assistance from A. Ferreira. Z.W., D.-K.K. and A.F.M. also gratefully acknowledge financial support from the Swiss National Science Foundation, the NCCR QSIT and the EU Graphene Flagship Project. A.H.M. and H.C. were supported by ONR-N00014-14-1-0330 and Welch Foundation grant TBF1473. H.C. and A.H.M. acknowledge the Texas Advanced Computing Center (TACC) at The University of Texas at Austin for providing HPC resources for the ab initio calculations in this work. H.C. thanks Y. Araki, X. Li and A. Da Silva for valuable discussions.

Author information

Affiliations

  1. Department of Quantum Matter Physics (DQMP) and Group of Applied Physics (GAP), University of Geneva, 24 Quai Ernest–Ansermet, CH1211 Genéve 4, Switzerland

    • Zhe Wang
    • , Dong–Keun Ki
    •  & Alberto F. Morpurgo
  2. Department of Physics, The University of Texas at Austin, Austin, Texas 78712, USA

    • Hua Chen
    •  & Allan H. MacDonald
  3. Institut de Physique de la Matière Complexe, Ecole Polytechnique Federale de Lausanne, CH–1015 Lausanne, Switzerland

    • Helmuth Berger

Authors

  1. Search for Zhe Wang in:

  2. Search for Dong–Keun Ki in:

  3. Search for Hua Chen in:

  4. Search for Helmuth Berger in:

  5. Search for Allan H. MacDonald in:

  6. Search for Alberto F. Morpurgo in:

Contributions

Z.W. fabricated the devices and performed the measurements with the collaboration of D.-K.K., under the supervision of A.F.M.; H.B. provided the WS2 crystals used to realize the devices; Z.W., D.-K.K. and A.F.M. analysed the data; H.C. performed the numerical calculations under the guidance of A.H.M.; all authors discussed and interpreted the results, and contributed to writing the paper.

Competing interests

The authors declare no competing financial interests.

Corresponding author

Correspondence to Alberto F. Morpurgo.

Supplementary information

PDF files

  1. 1.

    Supplementary Information

    Supplementary Figures 1-5, Supplementary Notes 1-7 and Supplementary References

Comments

By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.

Creative Commons BYThis work is licensed under a Creative Commons Attribution 4.0 International License. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in the credit line; if the material is not included under the Creative Commons license, users will need to obtain permission from the license holder to reproduce the material. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/