Layered antiferromagnets are rapidly garnering significant interest as a fertile set of materials to examine the interplay between magnetism and dimensionality, with promise in spintronics and twistronics applications1,2,3. Rare-earth tritellurides (RTe3, R = La, Ce, Pr, Nd, Sm, Gd, Tb, Dy, Ho, Er, and Tm) are one such class of materials whose magnetic and electronic characteristics have been the focus of a large body of research for more than two decades1,4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22,23,24. This class of van der Waals materials hosts an interesting unidirectional incommensurate charge density wave state with magnitude \(|{{\boldsymbol{q}}}_{{cdw}}|\approx \frac{2}{7}{q}_{b}\)6,8 (where \({q}_{b}=\frac{2\pi }{b}\); b is the lattice constant, space group is Bmmb) which is smoothly tunable by substitution of the different rare-earth elements25. In addition, all members of the series except LaTe3 and TmTe3 are magnetic, with each of the members aside from LaTe3, TmTe3, and ErTe3 ordering antiferromagnetically above 2 K25,26,27,28. While Fermi surface nesting had been assigned as the primary cause of the CDW in earlier work6,29,30, more recent studies7,31 indicate that the CDW formation is driven by strongly momentum-dependent electron-phonon coupling. The quasi-two-dimensional structure, consisting of RTe blocks separated by two Te square-lattice sheets on either side, is imprinted on the material’s electronic and magnetic characteristics. The itinerant electrons that initiate the CDW transition are mainly confined to the Te planes. However, since any magnetism comes from the rare-earth atoms, the magnetic moments reside on the RTe block. The physical separation between the localized and itinerant electrons can lead to multiple magnetic ground states and offers a valuable opportunity to examine the interplay between the charge order and magnetic order in these materials27,32,33,34,35,36,37,38,39,40,41,42,43,44,45,46.

Over the last three years, one member of the RTe3 family, GdTe3, has attracted significant attention for having the highest mobility of any van der Waals layered magnet, opening up possible applications in low-temperature spintronics devices as both an antiferromagnetic exchange layer as well as a highly conducting electrode in magnetic tunnel junctions1. The material exhibits superconductivity under pressure47 and recent measurements have suggested that the CDW ordering, with TCDW = 378 K, may be unconventional, based on the angular dependence of its Raman-scattering mode9,18,48. Previous measurements1,25,49 have shown a cascade of low temperature transitions in the specific heat and resistivity at ~12 K, ~10 K, and ~7 K which are also observed in magnetic susceptibility, suggesting that the system passes through a series of magnetic phases. However, despite the rapidly growing interest in this material, the exact nature of the magnetic phases in GdTe3 remains unknown in part because the large absorption cross-section of Gd makes neutron scattering measurements difficult11,40.

In this work, we use spin-polarized scanning tunneling microscopy (SP-STM) to investigate the low temperature magnetic states and the interplay between the CDW order and magnetic order in GdTe3. We note here the spin orders in this paper (unless specified otherwise) henceforth refer to the in-plane (2D) projection of the 3D order, which is what we measure with STM. Fourier transforms of STM topographies obtained with spin-polarized tips show new peaks not observed with normal (spin-averaged) tips. This allows us to determine that the magnetic ground state is a striped antiferromagnetic (AFM) phase with \({{\boldsymbol{q}}}_{{AFM}}=\left(\pm \frac{\pi }{a},0\right)\). By tracking the temperature evolution of the AFM and CDW peaks in the Fourier transforms we discover an unusual intermediate temperature magnetic order: a spin density wave (SDW) state with the same wave vector as the CDW.

Our data are best explained by the existence of an intermediate phase where the bulk Gd moments are ordered antiferromagnetically along the c-axis. This c-axis AFM order magnetically polarizes the electrons that make up the CDW, leading to a “daughter” SDW order in the bulk with wave vector equal to the sum of the c-axis AFM and CDW wave vectors. Since the c-axis AFM wave vector is normal to the surface, the SDW and CDW orders have the same wave vectors on the surface, as we observe. We present a Ginzburg-Landau theory that shows how this coupling between the magnetic and charge orders can lead to the SDW phase. Finally, our measurements establish a new method for uncovering such “hidden” order (i.e., a spin order with the same wave vector as the CDW) by comparing the temperature dependence of STM data obtained with spin-averaged and spin-polarized tips (details on the tips we use are given in the Methods section).


Spin-polarized STM measurements

A schematic of the GdTe3 lattice structure which consists of GdTe blocks separated by two Te square-lattice sheets is shown in Fig. 1a. The lattice constants a and b are nearly equivalent with a nominal value of 4.33 Å. A slight orthorhombicity in GdTe3, as is the case for every member of the RTe3 series, causes a ~0.1% difference between a and b with the CDW vector parallel to the longer direction; we assign this direction as b. The c direction lattice constant is 25.6 Å. The top view schematic in Fig. 1a shows the GdTe surface seen in our images. Only one species of atoms (either Te or Gd) is visible in most scans with a periodicity consistent with the Te/Gd lattice on the GdTe plane. Rarely however, both species are visible as shown in the inset to Fig. 1c. Another STM group, in Lee, et al. 23, has shown similar topography as in this inset, but reported cleaving between the two Te-only planes. However, given that we typically image a lattice with periodicity consistent with either the Gd or the Te atoms from the GdTe plane and given that we can image the magnetic order, we determine it to be more likely that we are measuring the Gd atoms on the GdTe plane.

Fig. 1: Crystal Structure, Fermi Surface, Topography, and dI/dV Spectra.
figure 1

a Crystal structure of GdTe3, with a top view of the GdTe surface shown to the right. b Sketch of Fermi surface. The shaded areas are a schematic representation of Fermi surface gapping associated with the unidirectional CDW. c Large-area (800 Å × 800 Å, VBias = −120 mV, ISet = 240 pA) and atomic-resolution (top right inset, 6 Å × 3.75 Å, VBias = −400 mV, ISet = 120 pA) topographies of cleaved GdTe3. All topographies in this manuscript are shown with a linear plane subtracted. d FT of the large-area W tip scan in c, with the CDW and Bragg peaks labeled as well as quasiparticle interference (QPI) bands observed. The QPI bands in the CDW direction (along qb) are gapped out. This FT has been mirror-symmetrized and had a first nearest-neighbor averaging applied. e Line profile along the blue arrow shown in d. The x-axis is the length in Fourier space in units of (2π/b). All data shown in this figure were taken at 4 K.

The unidirectional CDW is clearly visible as stripes in STM images taken with a metallic W tip as shown in Fig. 1c. The Fourier transform (FT) of this scan shows that the CDW wavevector is approximately 0.288 of the Bragg wavevector, which is close to a commensurate value of 0.286 (2/7). This suggests that the CDW in GdTe3 is very close to commensurate, similar to what was seen in a previous STM study of the related compound TbTe310; a closer examination is shown in Supplementary Fig. 1. FTs of our scans show strong quasiparticle interference bands (Fig. 1d, Supplementary Fig. 2). The bands are notably most prominent perpendicular to the CDW direction due to the CDW gapping out parts of the Fermi surface (Fig. 1b) along the CDW direction. A linecut along the CDW direction of our Fourier transforms (Fig. 1e) shows the CDW at the previously reported position \({{\boldsymbol{q}}}_{{CDW}} \sim \left(0,\pm \frac{2}{7}{q}_{b}\right)\) along with the expected satellite peaks. dI/dV spectroscopy (Fig. S3) measured between -400 meV and +400 meV shows changes in slope at -210 meV and +210 meV which have been attributed to the edges of the charge density wave gap in previously published data1,10.

Our next step is to determine the spin orders of the magnetic phases in GdTe3. To do this we use magnetic Cr tips which enable us to image spin contrast (schematic in Fig. 2a). The spin-polarization of our tips is confirmed by imaging the antiferromagnetically-ordered Fe1.03Te before obtaining measurements on GdTe3, as shown in Fig. S4. Figure 2b, c shows a topography and the corresponding FT of GdTe3 scanned with a Cr tip at a temperature of 4 K. Apart from the Bragg and CDW peaks seen in the W tip data, we observe two additional peaks whose wave vectors are independent of energy (Supplementary Fig. 5), as marked by the white triangle in Fig. 2c. As these peaks, found in every case of more than five distinct Cr tip and GdTe3 sample combinations (Supplementary Fig. 5) are only present when scanning GdTe3 with a magnetic Cr tip (comparison in Supplementary Fig. 6), they must be associated with magnetic ordering in the samples. These new peaks occur at precisely half the Gd Bragg peak wave vector and appear along only one lattice direction (Fig. 2f) and not the other (Fig. 2g), indicating that the spins order into a commensurate striped antiferromagnetic (AFM) phase with \({{\boldsymbol{q}}}_{{AFM}}=(\pm \frac{\pi }{a},0)\). This spin order can be seen in real space by carrying out the inverse FT of the lattice and AFM peaks as shown in Fig. 2d. Given existing evidence from magnetization measurements1 as well as density functional theory calculations50 that the spins in GdTe3 order in the ab-plane at low temperature, we conclude that the low temperature phase is an in-plane, striped AFM order as illustrated in Fig. 2e.

Fig. 2: Striped Antiferromagnetic Ordering in GdTe3.
figure 2

a Schematic of spin-polarized STM. b 80 Å × 80 Å topography of GdTe3 with a spin-polarized Cr tip (VBias = −200 mV, ISet = 280 pA). c FT of the GdTe3 scan with a spin-polarized Cr tip in b, showing Bragg peaks, CDW peaks, and an extra pair of peaks transverse to the CDW, arising due to commensurate striped antiferromagnetic (AFM) ordering. A first nearest-neighbor average has been applied to the FT. d Fourier-filtered scan by combining Bragg and AFM Fourier peaks, showing a square lattice, with striped AFM order; the Fourier transform used for filtering is that shown in c. The AFM intensity was multiplied by a factor of 5 for clearer visualization. e A zoom-in of the boxed region in d with positions of Te and Gd atoms displayed, along with a schematic of the spin order. f Line profile along yellow line in c, showing the AFM peaks at exactly half the Bragg peak distance; y-axis is normalized to the maximum Fourier amplitude and x-axis is length in Fourier space in units of (2π/a). g Line profile along green line in c, displaying CDW and satellite peaks, with y-axis normalized to the maximum Fourier amplitude and x-axis in units of (2π/b). Notably, there is no peak at half the Bragg peak distance as found in f; hence, the antiferromagnetism is a commensurate stripe order. h 1500 Å × 300 Å topography (VBias = −60 mV, ISet = 60 pA) across a CDW domain wall in GdTe3. Topography insets show high resolution 100 Å × 100 Å scans on either side of the domain wall; parameters are VBias = −60 mV, ISet = 60 pA. FTs of the inset topographies show the CDW direction rotating, along with a simultaneous rotation of the transverse antiferromagnetic peaks. This shows that the CDW and commensurate AFM ordering in GdTe3 always form transverse to one another. All data shown in this figure were taken at 4 K.

Interestingly, we find that qAFM always appears transverse to qCDW. This is exemplified by measurements across a domain wall (Fig. 2h, dI/dV map across domain wall in Supplementary Fig. 7) where the CDW order rotates by 90°. We note that the faint secondary stripe associated with the domain wall is not due to a tip effect and is rather a part of the structure of the domain wall and has been seen with other tips on other samples as shown in Supplementary Fig. 8. FTs of the topographies far from the domain wall show that the magnetic ordering flips by 90° across the boundary, concomitantly with the charge order (Fig. 2h). This demonstrates directly that the magnetic and charge orders form transverse to another. In addition, the domain wall brings another surprise. A closer look at the vicinity of the domain wall (Supplementary Figs. 9-10) shows the presence of a bidirectional CDW accompanied by a bidirectional AFM order on both sides of the domain wall. This is clearly visible in the topography as well as the FTs in the vicinity of the domain wall. Indeed, linecuts of the FT of these topographies along the two directions (Supplementary Figs. 9-10) now show the CDW and AFM peaks in both directions. As we move away from the domain wall, the region of coexistence eventually gives way to the regular unidirectional CDW and AFM orders. This can be confirmed by taking similar linecuts of FTs in areas far from the domain wall, which now show only the unidirectional CDW and the corresponding unidirectional AFM peaks (Supplementary Figs. 11-12) in the perpendicular direction. This observation is further strengthened by an amplitude map of the two CDW orders which shows that the two CDWs at the domain wall have nearly the same amplitude (Supplementary Fig. 13). The observation of bidirectional CDW and AFM orders is intriguing and has a few implications. First, the presence of a bidirectional CDW suggests that the area near the domain wall may be locally strained. This agrees with recent measurements in TbTe3 and ErTe320,21 where relatively small applied uniaxial strain was shown to not only flip the CDW direction but to also create a region of coexistence of the two perpendicular CDW orders. Second, the AFM order appears robust against the gapping of the Fermi surface which should now occur in both directions due to the presence of the bidirectional CDW. This may indicate that the Fermi surface does not play a critical role in the establishment of the antiferromagnetic order.

We next move ahead to the temperature evolution of the AFM order. As shown in Fig. 3a–d, the antiferromagnetic Fourier peaks, marked by white triangles, weaken noticeably with increasing temperature; by 7.9 K, the peaks are entirely gone (FT in Fig. 3c; temperature-dependent topographies in Supplementary Fig. 14). Upon cooling the sample again, the peaks recover as shown from the 4.7 K scan Fourier transform in Fig. 3d; more extensive Fourier transforms are shown in Supplementary Fig. 15. This evolution can be visualized in the inverse Fourier transforms combining the Bragg and antiferromagnetic peaks shown in Fig. 3e–g. A plot of the intensity of the AFM peak in the FT as a function of temperature shown in Fig. 3h captures this transition. The AFM peak intensity drops below the background by 7.9 K which suggests that the Néel temperature for the striped AFM order is ~7.5 K. This is several degrees lower than the first magnetic transition seen in susceptibility data at ~11.5 K and immediately raises the question: what is the magnetic order that emerges at 11.5 K? We address this question next.

Fig. 3: Temperature Dependence of Antiferromagnetism on GdTe3.
figure 3

ad FTs of AFM Fourier peaks from Cr tip scans at VBias = -400 mV, ISet = 60 pA on GdTe3 (topographies shown in Supplementary Fig. 14) show strong peaks at 4.4 K, a weaker peak at 6.7 K, and the absence of AFM peaks when heated to 7.9 K and above; cooling back down shows clear AFM peaks at 4.7 K. The displayed FTs have been first nearest-neighbor averaged. eg Inverse FTs of Bragg and AFM peaks from a to c show the decay of the magnetic order upon heating; the AFM Fourier intensity was multiplied by 5 to show the contrast more clearly. h Plot of the temperature dependence of AFM Fourier peak intensity, normalized to the maximum intensity value. The blue curve is a guide to the eye. The light gray line is a measure of the error given by the average background intensity level, with its thickness corresponding to the standard deviation of the background Fourier intensity.

Shown in Fig. 4a is the intensity of the CDW peak (ICDW) in the Fourier transform of our Cr tip topographies (shown in Supplementary Fig. 14) as a function of temperature. Intriguingly, we find that ICDW has a distinct temperature dependence only when measured with a Cr tip. As the sample is cooled below 12 K, ICDW increases, reaching a maximum at ~10 K, before rapidly decreasing back to the initial intensity between 7 and 8 K, as shown in Fig. 4a, c. This behavior is consistently reproducible as shown in Supplementary Fig. 16 which plots data from two more independently cleaved samples, each measured with a different Cr tip. In stark contrast, the intensity of the CDW peak in the FT of topographies taken with a non-magnetic W tip shows no systematic temperature dependence, as shown in Fig. 4b and Supplementary Figs. 17 and 18. The fact that the dI/dV spectra measured at 4.4 K, 9.9 K, and 13.9 K are nearly identical, as shown in Fig. 4d, rules out an electronic origin for this unusual temperature dependence.

Fig. 4: Evolution of Magnetic Ordering with Temperature.
figure 4

a CDW peak intensities from FTs of scans on GdTe3 taken with a spin-polarized Cr tip at VBias = -400 mV, ISet = 60 pA, as a function of temperature (topographies shown in Supplementary Fig. 14); y-axis normalization is to the maximum Fourier amplitude in the Cr tip run. Three distinct regimes are observed: a low-temperature region below 7 K in which the intensities are constant, an intermediate temperature phase between 7 K and 12 K where the intensities are considerably larger, and a high temperature region in which the intensities return to approximately the same, constant intensity as found below 7 K. Red points were taken on the temperature upsweep, while blue points were taken on the down sweep. b CDW peak intensities from FTs of GdTe3 scans taken with a spin-degenerate W tip at VBias = -240 mV, ISet = 240 pA, as a function of temperature (topographies shown in Supplementary Fig. 18), with y-axis normalization to the maximum Fourier amplitude in the W tip run. The intensities stay approximately constant, and any changes are random. c Linecuts along the CDW direction from FTs of the temperature-dependence, cropped to show the area around the CDW peak (highlighted by the shaded region). The CDW peak intensity significantly increases in the intermediate temperature regime. d Representative dI/dV spectra taken with a W tip on GdTe3 in each of the 3 temperature regimes; the electronic density of states is nearly identical, providing further evidence that the pattern in a is due to magnetic ordering. Setpoint for dI/dV spectra are VBias = -600 mV and ISet = 60 pA. e Schematic illustrating how the interaction between CDW order and ferromagnetic (FM) order would result in a daughter spin density wave order, represented by the spins of varying magnitudes in the bottom row.


An enhanced CDW Fourier peak intensity in an intermediate temperature range that is only observed with a spin-polarized tip indicates that there is a spin order with the same wave vector as the CDW. We henceforth refer to the spin order with the same wave vector as the CDW as the spin density wave (SDW). As the sample is cooled, the SDW sets in near 12 K and disappears between 7 K and 8 K. Below ~7.5 K, the striped AFM order described earlier emerges. We first consider the formation of the SDW near 12 K. There are several possible explanations for the formation of this SDW. It could, for example, be an independent magnetic order that forms near 12 K and coexists with the CDW. However, the fact that the SDW and CDW have the same wave vector would require fine tuning and renders this explanation unsatisfactory.

A more satisfactory explanation is that the SDW order occurs as a daughter order of the CDW order and an independent magnetic order that forms near 12 K. This other order could theoretically be a ferromagnetic order or an AFM order with a wave vector parallel to the c-axis, but only the formation of a c-axis AFM order near 12 K is consistent with bulk susceptibility and specific heat measurements1,49. As we show below, the combination of c-axis AFM and CDW orders would produce a daughter SDW order with wave vector equal to the sum of the c-axis AFM and CDW wave vectors. Since the c-axis AFM wave vector is normal to the ab-plane, the SDW and CDW have the same in-plane wave vector, without fine tuning. This can also be understood from the fact that, for a single ab-plane, the c-axis AFM is effectively a ferromagnetic order. This ferromagnetism imprints on the CDW, leading to a periodic modulation of the electronic spins with the same period as the CDW in each plane as illustrated in the schematic shown in Fig. 4e.

In the daughter SDW scenario, GdTe3 near the 12 K transition is described by the following minimal Landau free energy,

$$\begin{array}{c}F={m}_{c}{\left|{\bf{S}}_{\bf{{q}^{c}}}\right|}^{2}+{\lambda }_{c}{\left|{\bf{S}}_{\bf{{q}^{c}}}\right|}^{4}+{m}_{\rho }{\left|{\rho }_{\bf{Q}}\right|}^{2}+{\lambda }_{\rho }{\left|{\rho }_{\bf{Q}}\right|}^{4}+{m}_{{SDW}}{\left|{\bf{S}}_{{\bf{Q+q}}^{\bf{c}}}\right|}^{2}\\ +g\,{\bf{S}}_{{\bf{Q+q}}^{\bf{c}}}^{* }\cdot {\bf{S}}_{\bf{{q}^{c}}}{\rho }_{\bf{Q}}+{Higher}-{Order\; Corrections}\end{array}$$

where, ρQ is the CDW order parameter with wave vector \({\bf{Q}}\,\approx\, (0,\frac{2}{7}{q}_{b},0),{\bf{S}}_{\bf{{q}^{c}}}\) is the c-axis AFM order parameter with wave vector qc, and \(\bf{{S}_{{Q+q}^{c}}}\) is the SDW order parameter with wave vector Q + qc. The simplest case is a period-2 c-axis AFM, where \(\bf{{q}^{c}}=\left(\mathrm{0,0},\frac{\pi }{c}\right)\), but our conclusions are independent of the exact value of qc. If the quadratic terms, \({m}_{c},{m}_{\rho },\) and mSDW, are negative (positive) the corresponding order parameter has (does not have) an expectation value. The λc, and λρ terms are the standard quartic Landau terms needed for stability, when \({m}_{c},{m}_{\rho }\) are negative. As we shall discuss momentarily, it is not necessary to include a quartic term for \(\bf{{S}_{{Q+q}^{c}}}\) in our immediate analysis, and we shall therefore leave it implicit in the “Higher-order Corrections.” We additionally have the non-trivial tri-linear g term, which couples the CDW, c-axis AFM, and SDW order parameters. Physically, this term describes how the wavevector Q charge density wave can imprint on the wavevector qc spin density wave, leading to additional spatial oscillations of the spins with wavevector Q + qc. We are interested in the situation where the c-axis AFM order develops below \({T}_{c}\sim 12K\), which corresponds to setting \({m}_{c}=\alpha (T-{T}_{c})\) for some α > 0. Since the CDW order develops at much higher temperatures, we use a constant value of \({m}_{\rho }, \,< \,0\) such that \({\langle \rho }_{Q}\rangle \,\ne \,0\). We also set \({m}_{{SDW}} \,> \,0\), such that an independent \(\bf{{S}_{{Q+q}^{c}}}\) SDW order does not form near 12 K. Because we are only considering mSDW > 0 the Landau free energy is stable without including a quartic term for \(\bf{{S}_{{Q+q}^{c}}}\). We have not included all symmetry-allowed terms here; notably, we are missing biquadratic terms that promote the coexistence of different ordering. However, this minimal free energy is sufficient to capture how a daughter SDW order can arise from the combination of c-axis AFM and CDW orders.

For T < Tc, there is c-axis AFM order, \(\langle \bf{{S}_{{q}^{c}}}\rangle\, \ne \,0\). Because of the tri-linear g term, the free energy is minimized when the SDW order also has an expectation value, \(\langle {{\bf{S}}_{{Q+q}^{c}}}\rangle =-\frac{g}{{m}_{{SDW}}}\langle {{\bf{S}}_{{q}^{c}}}\rangle {\langle \rho }_{\bf{Q}}\rangle\) for \(T\, < \,{T}_{c}\). The combination of CDW order, \({\langle \rho }_{\bf{Q}}\rangle\, \ne \,0\), and c-axis AFM order, \(\langle \bf{{S}_{{q}^{c}}}\rangle \,\ne \,0\), therefore produces a daughter SDW order, \(\left\langle \bf{{S}_{{Q+q}^{c}}}\right\rangle\, \ne \,0\), as discussed above. It is worth stating explicitly that the above Landau free energy only describes the system near the 12 K transition, and does not capture the magnetic transition that occurs near 7.5 K.

We next turn our attention to the disappearance of the SDW and formation of the striped AFM that occurs near 7.5 K. A simple scenario to explain the low temperature phase is that the c-axis AFM present between 7.5 K and 12 K rotates to the ab-plane below 7 K where it becomes the striped AFM that we observe. The interplay between the low temperature and the intermediate phase orderings is presumably due to competing interactions. Alternatively, it could be the case that the c-axis and striped AFM phases are separated by a small paramagnetic phase. This would mean that there is a reentrant phase transition near 7.5 K that is likely driven by entropy effects44,45. Finally, the c-axis and striped AFM phases could simply be directly connected via a first-order phase transition1.

Using spin-polarized STM, we have thus identified the in-plane low temperature magnetic phases of GdTe3. Our data show that there are two distinct magnetic orders – an emergent spin density wave with wave vector \({{{\boldsymbol{q}}}_{{SDW}=}{\boldsymbol{q}}}_{{CDW} \sim }(0,\pm \frac{2}{7}{q}_{b})\) that sets in at ~12 K and likely coexists with a c-axis AFM order, and a striped antiferromagnetic order with wave vector \({{\boldsymbol{q}}}_{{AFM}}=(\pm \frac{\pi }{a},0)\) that sets in at ~7.5 K. We propose that the SDW occurs as a daughter order of an intermediate temperature c-axis AFM phase and the CDW, while the striped AFM is the actual low temperature ground state. Through this work, we have also demonstrated how comparing the temperature dependence of Fourier transform intensities measured with spin-polarized and spin-averaged STM tips enables the detection of hidden spin orders that may have the same periodicity as different orders in the system. Future experiments with SP-STM on the rare-earth tritellurides in the presence of an in-plane magnetic field could provide further evidence elucidating the complex interplay between magnetic and charge orders in this distinctive class of materials.


Crystal growth, STM measurements, and data processing

GdTe3 single crystals were grown by a self-flux technique, as reported previously25,29,51; crystals used in this work have approximate dimensions of 2 mm × 2 mm. STM measurements were performed after cleaving single crystals of Fe1.03Te and GdTe3 at 77 K. W tip wires of 250 μm diameter and Cr tip wires of 300 μm diameter are used for measurements. W tips are electrochemically etched in an NaOH solution, while Cr tips are electrochemically etched using H2SO4. Additional data with a W tip is shown in Supplementary Figs. 17, 18, and 19. Both types of tips are annealed in vacuum prior to measurements. Cr tips are used for the spin-polarized measurements described, and are calibrated on antiferromagnetic Fe1.03Te single crystals, as shown in a number of previous works18,26,38,52,53. Example calibration is shown in Fig. S4 and examples of the robustness of maintaining spin-polarization in Cr tips while changing samples are shown in Supplementary Fig. 20. For scanning tunneling spectroscopy, a Stanford Research Systems SR830 lock-in amplifier is used, with dI/dV spectra obtained at a lock-in frequency of 913 Hz. To perform temperature dependence measurements, we employ Joule heating with a Cu coil; the temperatures are set and maintained with a Lakeshore 340 controller. Fourier peak intensities are extracted by taking the average intensity value of a 3 × 3-pixel area centered on the peak. Background intensity is determined by taking the average intensity of a 3 × 3-pixel area in a region of the Fourier transform far from any peaks. The intensity of the centermost pixels of Fourier transforms is suppressed so they don’t dominate the color contrast. In the limited cases where Fourier transforms have been mirror-symmetrized, we have explicitly noted this step in the caption; while features of the Fourier transform are occasionally clearer visually after this step, the Bragg peaks, CDW peaks, and quasiparticle interference patterns are visible even without this processing and the mirror-symmetrization does not affect our conclusions.