Introduction

A fundamental assumption of the Bardeen–Cooper–Schrieffer (BCS) theory of superconductivity is that two electrons form a Cooper pair with zero center-of-mass momentum. Realizing exotic superconducting states with finite-momentum pairs that violate this assumption has been a long-sought goal in condensed matter physics. Such a superconducting state is an enticing theoretical possibility but has proven a severe experimental challenge. This is not only because the conditions under which such a superconducting state can be formed are rather stringent but also because smoking-gun experiments to confirm its existence have still been lacking.

Helical superconductivity, in which the amplitude of the superconducting order parameter is constant, but its phase is spontaneously and spatially modulated, has been proposed as a prominent example of such a finite-momentum pair state1,2,3,4. The realization of helical superconductivity requires a strong Rashba effect that appears as a combined consequence of significant spin-orbit interaction (SOI) and spatial inversion symmetry breaking. When the crystal structure lacks a center of inversion, the SOI may dramatically change the electronic properties, leading to nontrivial quantum states. The key microscopic ingredient in understanding the physics of such noncentrosymmetric materials is the appearance of antisymmetric SOI of the single electron states. Asymmetry of the potential in the direction perpendicular to the two-dimensional (2D) plane ∇ V∥(001) induces Rashba type SOI, αRg(k) ⋅ σ ∝ (k × ∇ V) ⋅ σ, where αR is the Rashba coupling, k is the wave number, g = (−ky, kx, 0)/kF with kF the Fermi wave number, and σ is the Pauli matrix5. Rashba SOI splits the Fermi surface into two sheets with different spin structures. The energy splitting is given by αR, and the spin direction is tilted into the plane, rotating clockwise on one sheet and anticlockwise on the other.

The Rashba SOI has profound consequences on the superconducting states6,7. For example, parity is generally no longer a good quantum number, leading to exotic states with a mixture of spin-singlet and spin-triplet components. When the Rashba splitting becomes sufficiently larger than the superconducting gap energy, it has been theoretically proposed that an even more fascinating superconducting state may emerge in 2D superconductors by applying strong parallel magnetic fields; a conventional BCS state with zero-momentum pairs (k↑, −k↓) formed within spin-textured Fermi surfaces (Fig. 1a) changes into a superconducting state with finite-momentum pairs formed within each spin nondegenerate Fermi surface1,2,3,4 (Fig. 1b). Such a superconducting state appears as a result of the shift of the Rashba-split Fermi surfaces by external parallel fields. When the magnetic field is applied parallel to \(\hat{{{{{{{{\bf{x}}}}}}}}}\) axis (\({{{{{{{\bf{H}}}}}}}}=H\hat{{{{{{{{\bf{x}}}}}}}}}\)), the center of the two Fermi surfaces with different spin helicity are shifted along \(\hat{{{{{{{{\bf{y}}}}}}}}}\) axis in opposite directions. This state, referred to as a helical superconducting state, is characterized by the formation of Cooper pairs (k + qR↑, −k + qR↓), where \({{{{{{{{\bf{q}}}}}}}}}_{R}={\mu }_{B}H\hat{{{{{{{{\bf{y}}}}}}}}}/\sqrt{{\alpha }_{R}^{2}+\frac{2{E}_{F}}{m}}\) with Bohr magneton μB, Fermi energy EF and quasiparticle mass m. This pair formation leads to a state in which the magnitude of the superconducting order parameter is constant, while its phase rotates in space with period π/∣qR∣ as \({{\Delta }}({{{{{{{\bf{r}}}}}}}})={{{\Delta }}}_{0}{e}^{2i{{{{{{{{\bf{q}}}}}}}}}_{{{{{{{{\bf{R}}}}}}}}}\cdot {{{{{{{\bf{r}}}}}}}}}\).

Fig. 1: Schematic of the various types of Cooper pairings.
figure 1

a Conventional BCS pairing state. Zero-momentum pairing with (k↑, −k↓) occurs between electrons in states with opposite momentum and opposite spins. b Helical superconducting state. Arrows on the Rashba-split Fermi surfaces indicate spins. H parallel to \(\hat{{{{{{{{\bf{x}}}}}}}}}\) axis shifts the center of the small and large Fermi surfaces by qR along +y and −y directions, respectively. Pairs are formed within each Rashba-split Fermi surface between the states of (k + qR↑, −k + qR↓), leading to a gap function with modulation of phase \({{\Delta }}({{{{{{{\bf{r}}}}}}}})\propto \exp (2i{{{{{{{{\bf{q}}}}}}}}}_{{{{{{{{\bf{R}}}}}}}}}\cdot {{{{{{{\bf{r}}}}}}}})\). Cooper-pairs have finite center-of-mass momentum qR. c FF and LO pairing states. Pairing with (k + qZ↑, −k + qZ↓) occurs between sections of the Zeeman-split Fermi surfaces, where qZ ≈ 2μBH/ℏvF. Cooper-pairs have finite center-of-mass momentum qZ. In the FF state, the order parameter varies as \({{\Delta }}({{{{{{{\bf{r}}}}}}}})\propto \exp (2i{{{{{{{{\bf{q}}}}}}}}}_{{{{{{{{\bf{Z}}}}}}}}}\cdot {{{{{{{\bf{r}}}}}}}})\), while in the LO state, it varies as \({{\Delta }}({{{{{{{\bf{r}}}}}}}})\propto \cos (2{{{{{{{{\bf{q}}}}}}}}}_{{{{{{{{\bf{Z}}}}}}}}}\cdot {{{{{{{\bf{r}}}}}}}})\).

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We note that the helical state is essentially different from the Fulde–Ferrell (FF) and Larkin–Ovchinnikov (LO) states, in which finite-momentum Cooper pairs are formed between sections of the Zeeman-split Fermi surfaces8,9 (Fig. 1c). A potential FF or LO state has been reported in several candidate materials, by showing a phase transition inside the superconducting state10,11 through the measurements of magnetization12, specific heat13,14,15, nuclear magnetic resonance16,17,18, thermal conductivity19, ultrasound20,21, and scanning tunneling microscope22. In the FF state, the finite-momentum Cooper pairs lead to the phase modulation of the superconducting order parameter, which is difficult to detect directly. In the LO state, the spatial modulation of the superconducting order parameter due to such pairs gives rise to periodic nodal planes in the crystal. However, it should be emphasized that no direct evidence showing such periodic nodes has been reported so far. This is mainly due to the inherent challenge in directly measuring the momentum of Cooper pairs within a superconducting state, calling for a novel probe to investigate the Cooper pair momentum.

Very recently, it has been theoretically proposed that superconducting states with finite-momentum Cooper pairs exhibit a current-direction-dependent critical current, namely the superconducting diode effect23,24,25,26. This diode effect appears due to the nonreciprocal nature of the pair momentum-dependence of the free energy. In the framework of superconductivity, the superconducting current, denoted as j, and the center-of-mass momentum of Cooper pairs, represented by q, are coupled within the free energy expression as F ~ j ⋅ q. This coupling suggests that, analogous to how a magnetic field serves as a probe for investigating ferromagnetic properties, the superconducting current provides a robust means to probe the dynamics of the center-of-mass momentum of Cooper pairs. Notably, the diode effect is significantly enhanced upon entering the helical superconducting state both in s-wave24,26 and d-wave superconductors27. The enhancement naturally leads to characteristic behaviors of nonreciprocal electron transport (NRET) in general. Therefore, measurements of the NRET provide a powerful tool for revealing the helical superconductivity. The resistance of a 2D film can be described as \(R={R}_{0}(1+\gamma {\mu }_{0}{{{{{{{\bf{H}}}}}}}}\times \hat{{{{{{{{\bf{z}}}}}}}}}\cdot {{{{{{{\bf{I}}}}}}}})\), where R0 and I are the resistance in the zero-current limit and an electric current, respectively. The coefficient γ gives rise to different resistance for rightward and leftward electric currents and can be finite in noncentrosymmetric materials. Unless the resistive transition in magnetic fields is very sharp due to strong pinning, the NRET response can be obtained by measuring the second harmonic resistance R2ω. The comparison between R2ω at low frequencies in the DC limit and the differential in the critical current has been well-documented across various systems, and the general consensus is that if one is finite, the other will also be finite28,29.

NRET has been studied in several superconductors28,30,31. However, it remains an arduous task to discern whether the observed NRET response stems from intrinsic superconducting phenomena, such as exotic pairing states that contain finite-momentum Cooper pairs. This is because the NRET response can also arise from extrinsic effects such as asymmetric vortex pinning at the edge, surface, and interface, the ratchet effect of the pinning center, and geometry-dependent Meissner shielding effects32,33,34,35.

To address this challenge, we have developed tricolor Kondo superlattices composed of atomically thin CeCoIn5 layers. We have methodically isolated the intrinsic superconducting effects, thereby eliminating extrinsic influences. This approach has unveiled a nonreciprocal response that stems from the intrinsic superconducting properties characterized by the formation of finite-momentum pairs. We associate the observed high-field state with the helical superconducting state.

Results

Sample characterization

CeCoIn5 is a well-known heavy-fermion superconductor with the highest bulk Tc of 2.3 K, in which \({d}_{{x}^{2}-{y}^{2}}\) superconducting gap symmetry is well established36,37. Recently, using state-of-the-art molecular beam epitaxy (MBE) technology38, we have successfully fabricated epitaxial thin films of CeCoIn5 and atomic-thickness superlattices of CeCoIn5, alternating with layers of different materials39,40 such as CeIn341, CeRhIn542, YbRhIn543, and YbCoIn544,45. The epitaxial growth of these superlattices was confirmed by reflection high energy electron diffraction (RHEED). The interfaces between CeCoIn5 and adjacent layers are characterized by their distinct atomic sharpness, a feature confirmed through multiple methods. Specifically, both transmission electron microscopy (TEM) and electron energy loss spectroscopy (EELS) have substantiated this attribute42. In our TEM analyses, we verified the absence of texturing over micrometer-scale areas along the layer direction. Furthermore, scanning tunneling microscopy (STM) topographic images corroborate this finding; they reveal an atomically flat surface of the CeCoIn5 layers46,47, with no indications of texturing. This collective evidence strongly supports that the samples are indeed single-crystalline and devoid of any textural anomalies.

The bulk CeCoIn5 possesses the inversion center. Then, fabricating tricolor superlattices with an asymmetric ⋯A/B/C/A/B/C⋯ arrangement, in which non-superconducting metals sandwich CeCoIn5 with atomic layer thickness, we can introduce the global inversion symmetry breaking (Fig. 2a)39,40,43,48. Given that this superlattice comprises three distinct materials, it will be designated as tricolor henceforth. This tricolor system provides an ideal platform for revealing the helical superconducting state for the following reasons. First, Ce atoms have a large SOI, and the condition that the Rashba-SOI well exceeds the superconducting gap has been confirmed in various superlattices of CeCoIn5, including the present tricolor superlattice, by the highly enhanced upper critical field from Pauli limited critical fields in bulk (see SI and ref. 40). Second, Cooper pairs can be confined in atomic CeCoIn5 layers, forming 2D superconductivity48. Third is the strong electron correlation effect in CeCoIn5. It has been theoretically pointed out that the correlation further strengthens the effect of Rashba SOI49. Furthermore, the suppression of the orbital pair-breaking effects promotes the appearance of helical superconducting phases. These features make the CeCoIn5 superlattice system unique and suitable for realizing helical superconductivity compared to weakly correlated systems. Finally, d-wave superconductors are expected to respond differently to in-plane magnetic fields directed for the nodal and antinodal directions, possibly allowing the intrinsic NRET to be extracted by changing the field direction.

Fig. 2: Tricolor d-wave superconducting superlattices.
figure 2

a Schematic representation of noncentrosymmetric tricolor Kondo superlattices with ⋯A/B/C/A/B/C ⋯ structure. The sequence of YbCoIn5(3)/CeCoIn5(8)/YbRhIn5(3) is stacked repeatedly 30 times, so that the total thickness is about 300 nm. The orange arrows represent the asymmetric potential gradient ∇V, which gives rise to the Rashba splitting of the Fermi surface with different spin structures. The crystal structure of Ce(Yb)Co(Rh)In5 is also illustrated. b The scanning electron microscopy image of a tricolor superlattice patterned by focused ion-beam (FIB). The black line regime corresponds to the area cut by FIB. Red, blue, and green lines indicate the current path along [100], [010], and [110], respectively. The width of the current path is 20 ± 2 μm. c The temperature dependence of the dc-resistance Rdc for H∥[100] and I∥ [010].

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The tricolor superlattices with a c-axis-oriented structure have been epitaxially grown on an MgF2 substrate using the MBE technique. The structure consists of alternating layers: 3-unit-cell-thick (3-UCT) YbCoIn5, 8-UCT CeCoIn5, and 3-UCT YbRhIn5. In this configuration, YbCoIn5 and YbRhIn5 act as conventional non-superconducting metals (Fig. 2a). The deposition sequence of YbCoIn5/CeCoIn5/YbRhIn5 was repeated 30 times. Within these tricolor superlattices, none of the layers act as mirror planes, thereby introducing broken inversion symmetry along the stacking direction. It is noteworthy that the present superlattice structure, comprising 30 layers, significantly reduces the influence of the substrate, rendering it negligible for our experimental purposes. In addition, for comparison, we fabricated bicolor superlattices with ⋯A/B/A/B⋯ stacking structure, in which spatial inversion symmetry is preserved. In this superlattice, the deposition sequence of YbCoIn5 (5-UCT)/CeCoIn5 (8-UCT) was repeated 30 times.

Given the necessity for a precise in-plane application of the magnetic field in this study, we employed the 8-UCT CeCoIn5 tricolor superlattice sample previously characterized in ref. 48. This referenced work extensively investigated the temperature and angular dependence of the upper critical field for the sample. Since CeCoIn5 is a quasi-2D superconductor with a larger coherence length in the ab-plane (ξab) compared to along the c-axis (ξc), and the thickness of 8-UCT CeCoIn5 layers in the present superlattices is comparable to ξc, elliptical vortices are likely to form within these layers when exposed to a parallel field. Moreover, the presence of the strong Rashba SOI is confirmed by the suppressed Pauli limit48. For the sake of achieving a high current density and ensuring meticulous control over the current orientation, the sample underwent patterning utilizing a focused ion beam (FIB) as depicted in Fig. 2b. We note that both the Tc and upper critical field of this sample changed only slightly before and after FIB patterning (See Fig. S1). The sample becomes superconducting at Tc = 0.83 K defined as the temperature at which the dc-resistance Rdc drops to 50% of its normal state value at the onset (Fig. 2c). The observed decrease in Tc of the superlattice, compared to the bulk sample, can plausibly be attributed to the modification of the electronic band structure from 3D to 2D. This alteration leads to changes in the antiferromagnetic fluctuations, which play an essential role in the unconventional superconductivity of CeCoIn542. Nonreciprocal transport measurements are carried out by the standard lock-in technique (see Materials and Methods in SI). The R2ω curves are antisymmetrized with respect to a magnetic field. The misalignment of H from the ab plane is less than 0.05∘.

Nonreciprocal transport

Figure 3 depicts R2ω normalized by normal state resistance Rn when both in-plane H and I are applied to nodal (H∥[110], \({{{{{{{\bf{I}}}}}}}}\parallel [1\bar{1}0]\)) and antinodal (H∥[100], I∥[010]) directions (see the inset). NRET can manifest even in the normal state in the presence of inversion symmetry breaking. However, for both configurations, no discernible NRET is observed in high temperatures or high magnetic fields, indicating that the observed response purely arises from superconducting properties. Therefore, despite the broadening of resistive transition that the inhomogeneity may cause, only the superconducting response of R2ω can be extracted. For the nodal configuration, R2ω increases with H at low temperatures, peaking at μ0H ~ 6 T and disappearing at high fields. It should be noted that such a single-peak structure as a function of H in the superconducting state has also been observed in NbSe231 and ion-gated SrTiO330, in which peaks gradually shift and decrease as the temperature elevates. It was found that such a structure can be explained by the vortex motion. On the other hand, for the antinodal configuration, while a similar peak is observed at high temperatures, the peak is suppressed around μ0H ~ 5 T at low temperatures, exhibiting a distinct dip anomaly. While there may be an underlying structure at low magnetic fields, the signal is vanishingly small. Therefore, in this study, our focus is on the signals at high fields.

Fig. 3: Nonreciprocal electronic transport in the superconducting state of tricolor superlattice.
figure 3

The field dependence of second harmonic resistance R2ω normalized by Rn in tricolor superlattice for two configurations. Blue upper triangles show R2ω/Rn for both H and I applied parallel to the d-wave nodal direction (H∥[110], I∥[1\(\bar{1}\)0]), as illustrated by the left panel in the inset. Red lower triangles show R2ω/Rn for antinodal configuration (H∥[100], I∥[010], right panel in the inset). The curves are vertically shifted for clarity. The dashed lines indicate the baselines. The gray area represents the difference between the two configurations ΔR2ω/Rn. Arrows indicate Hc2∥ determined by Rdc.

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As noted above, finite R2ω originates from the Cooper pairs. There are two possible sources for the NRET response in the superconducting state. One is extrinsic origin such as Meissner screening current and vortex motion, and the other is intrinsic origin due to the exotic superconducting state with finite-momentum pairing. We here discuss extrinsic origins. The direction-dependent critical current can be induced by the combination of the Meissner screening effect and the asymmetric vortex surface barrier arising from the sample edges50. However, since such an effect is important only at a very low field around the lower critical field, it is negligibly small in the present field range, which significantly exceeds the Pauli limit.

Another extrinsic origin is the asymmetric vortex motion. When both H and I(⊥H) are applied in-plane, the vortices move in and out across the interfaces. If there is an asymmetric vortex pinning potential at the interface of the different materials, NRET may occur. In the tricolor superlattices, different vortex thread pinning potentials on either side of the superconductor interface may induce NRETs of different amplitudes, leading to an asymmetric motion that can generate a net NRET signal. To confirm this, we measured the NRET response in bicolor ⋯A/B/A/B ⋯ stacking superlattices with canceling contributions on both sides of the interface. Figure 4 depicts the NRET of the bicolor superlattice for the nodal (\({{{{{{{\bf{H}}}}}}}}| | [110],\, {{{{{{{\bf{I}}}}}}}}\parallel [1\bar{1}0]\)) and antinodal (H∣∣[100], I∥[010]) configurations. The figure includes the NRET of the tricolor superlattice in the nodal configuration for comparison. In the bicolor superlattice, the NRET is found to be absent or negligibly small, especially when compared to that of the tricolor superlattice. This supports the presence of the NRET response arising from vortex motion perpendicular to the layers. To rule out the possibility of pancake vortices perpendicular to the layer created by small but finite misalignment of H out of the 2D plane inducing the NRET effect, we measured the NRET by applying H tilted about 4∘ from the ab plane and found no such effect in the tricolor superlattices (See Fig. S4). Additionally, no NRET effect was observed in the Lorentz force-free geometry, H∥I. These results indicate that the extrinsic NRET response, if present, arises from asymmetric vortex motion perpendicular to the layers.

Fig. 4: Nonreciprocal electronic transport in the superconducting state of bicolor superlattice.
figure 4

For the bicolor superlattice, the sequence of YbCoIn5(5)/CeCoIn5(8) is stacked repeatedly for 30 times. The field dependence of second harmonic resistance R2ω normalized by Rn in bicolor superlattice for two configurations is shown. Red upper triangles show R2ω/Rn for both H and I applied parallel to the d-wave nodal direction (H∥[110], I∥[1\(\bar{1}\)0]). Black open circles show R2ω/Rn for antinodal configuration (H∥[100], I∥[010]). For comparison, R2ω/Rn for nodal configuration is also potted by Blue upper triangles. The curves are vertically shifted for clarity.

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We note that in the present tricolor superlattices, the vortex motion perpendicular to the 2D plane is almost independent of the in-plane directions of H and I(⊥H). This can be attributed to the following reasons: First, the superlattices with tetragonal crystal symmetry have no twin boundaries. Additionally, as illustrated in Fig. S1, the in-plane critical field Hc2 is almost isotropic. The electronic structure of a vortex is determined by its coherence length, which, in turn, is determined by the average of the Fermi velocity. Given that the coherence length is directly related to Hc2, an isotropic in-plane Hc2 suggests that the electronic structure of vortices for H∥ [100] is very similar to that for H∥ [110]. This isotropy in Hc2 is also reflected in the behavior of the electrical current, which is dependent on the Fermi velocity. Consequently, the uniformity of the average Fermi velocity within the plane implies an isotropic current contribution as well.

To separate the intrinsic contribution from the extrinsic one, we take the difference between two configurations, as represented by the gray area in Fig. 3. Notably, except for the gray area at low temperatures, R2ω from the two configurations nearly overlaps. This indicates that R2ω for both configurations is dominated by extrinsic vortex motion except for the regime where R2ω exhibits a dip anomaly at low temperatures around μ0H ~ 5 T for the antinodal configuration. Therefore, the dip anomaly when both H and I are applied to antinodal directions is attributed to an intrinsic origin arising from the Cooper pairs superimposed on the extrinsic vortex contribution. To obtain further information on the origin of the dip, R2ω was measured at different relative angles of H and I; H∥[100] and I∥[1\(\bar{1}\)0], and H∥[110] and I∥[010] (see SI for details). The results show that the appearance of the dip anomaly is determined by field direction, not by the current direction, implying that the dip anomaly is related to the superconducting gap structure.

Phase diagram

The NRET response provides pivotal information on the superconducting phase diagram of the tricolor superlattice displayed in Fig. 5. The solid line in Fig. 5 represents the upper critical field for H∥[100], Hc2∥, determined by H where Rdc reaches 50% of Rn. We find that Hc2∥ line for H applied nodal direction well coincides with that for antinodal direction, indicating a similar HT-phase diagram (Fig. S1). The upper right (colored in light brown) area in Fig. 5 represents the normal state. In the superconducting state below Hc2∥, the difference of R2ω between two configurations, \({{\Delta }}{R}_{2\omega }\equiv {R}_{2\omega }({{{{{{{\bf{H}}}}}}}}| | [110],\, {{{{{{{\bf{I}}}}}}}}| | [1\bar{1}0])-{R}_{2\omega }({{{{{{{\bf{H}}}}}}}}| | [100],\, {{{{{{{\bf{I}}}}}}}}| | [010])\), normalized by Rn, is plotted in color; the gray area displayed in Fig. 3 corresponds to ΔR2ω/Rn. In the light blue area at low fields in Fig. 5, while finite R2ω is observed for both configurations due to extrinsic contributions from vortex motion, ΔR2ω is negligibly small. In the red area at high fields, the finite ΔR2ω appears due to the intrinsic contribution originating from Cooper pairs. Note that as shown by arrows in Fig. 3 indicating Hc2∥ determined by Rdc, ΔR2ω vanishes at around Hc2∥, while small but finite R2ω remains at Hc2∥, likely due to the superconducting fluctuation effect and inhomogeneity.

Fig. 5: Superconducting phase diagram of the tricolor superlattice determined by nonreciprocal electron transport properties.
figure 5

The solid line is Hc2∥ determined by Rdc. Hc2∥ line for nodal and antinodal directions well coincides each other. The light brown area represents the normal regime. In the superconducting state, the difference of R2ω/Rn between two configurations, ΔR2ω/Rn, is plotted in color. The blue area at low fields represents the BCS regime, where ΔR2ω/Rn is negligibly small while finite R2ω is observed for both configurations due to extrinsic contributions from vortex motion. The red area at high fields corresponds to the helical superconducting state, where the finite ΔR2ω/Rn appears due to the intrinsic contribution originating from Cooper pairs.

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In the bicolor system where the NRET is not observed, no discernible difference is observed between the antinodal and nodal configurations (Fig. 4}. The fact that the bicolor superlattice preserves global inversion symmetry leads us to conclude that the emergence of NRET difference in the tricolor lattice, ΔR2ω, is an intrinsic phenomena arising from the Rashba SOI. The intrinsic NRET emerges as a direct consequence of the state with finite-momentum pairs, and such an effect is negligibly small in the BCS state. Therefore, the results of Fig. 5 provide evidence for the appearance of a high-field superconducting state at the low-T/high-H corner, distinct from the low-field BCS state. Although the anomalous upturn behavior of Hc2∥ at low temperatures has been suggested in the previous study48, the superconducting state at high fields had remained an unresolved issue, including the possible existence of a new phase. We note that we can rule out the possibility that the observed nonreciprocal phenomena are tied to the so-called Q-phase51, in which the superconductivity may be intertwined with magnetic order, in bulk CeCoIn5 for the following reasons. Firstly, in the basic Drude model, nonreciprocal transport is independent of spin. Then, the primary effect of the Q-phase on nonreciprocal transport is the Brillouin zone folding, but this has a negligible effect. In addition, in the Q-phase, where spatial modulations of order parameters appear, electron scattering should increase, resulting in the suppression of the nonreciprocal response. However, our observations indicate the opposite in the current case. Furthermore, Cooper pairs in the Q-phase do not carry a finite momentum. Hence, even when the inversion symmetry is broken, the momentum of the Cooper pair remains unchanged.

As discussed above, the NRET is caused purely by the supercurrents, which directly couple to the finite momentum Cooper pairs. It is crucial to clarify why the nonreciprocal signal is strongly suppressed in the normal state, despite the presence of broken inversion symmetry. This suppression can be attributed to the fact that the signal is proportional to 1/EF in the normal state and to 1/Δ in the superconducting state, where EF and Δ represent the Fermi energy and the superconducting gap, respectively. Consequently, the signal is significantly smaller in the normal state52,53.

In the context of magnetic field-induced resistive transitions in superconductors, particularly when the transition is broadened due to superconducting fluctuations as observed in this study, there is a degree of uncertainty in selecting the appropriate resistance threshold (0.9 Rn, 0.5 Rn, or 0.1 Rn) to define the mean-field upper critical field. However, given that NRET is vanishingly small in the normal state, it is natural to associate the mean-field upper critical field with the emergence point of observable NRET. In the present case, the magnetic field corresponding to 0.5 Rn closely aligns with this emergence point. Consequently, this value has been adopted to define the mean-field upper critical field. It is worth noting that the intrinsic contribution of NRET predominantly becomes discernible in the resistance range between R = 0.1Rn and R = 0.5 Rn as shown in Fig. S5.

Discussion

It should be emphasized that we can discard the possibility of both FF and LO states10 (Fig. 1c), where pairing between sections of the Zeeman-split Fermi surfaces results in Cooper-pairs (k + qZ↑, −k + qZ↓) with momentum qZ ≈ μBH/ℏvF (vF is the Fermi velocity), as the origin of the intrinsic NRET phenomena. This is because the energy of the Rashba spin splitting is overwhelmingly larger than the superconducting gap energy in the present tricolor superlattices, as demonstrated in ref. 48 (see Fig. S2). In this situation, FF- and LO-type pair formation cannot occur. In the absence of inversion symmetry, the LO phase can be characterized by a general order parameter, formulated \(a{e}^{2i{q}_{Zr}}+b{e}^{-2i{q}_{Zr}^{{\prime} }},\, a \, \ne \, b\). This phase, as defined by the order parameter, is commonly referred to as the “stripe phase”. However, theoretical predictions suggest that the stripe phase only emerges within a narrow region at low temperatures in the HT-phase diagram2, whereas helical superconductivity manifests within a more expansive phase region surrounding it. Considering this, it seems plausible that our experimental observations represent helical superconductivity. It may be possible, however, to observe a stripe phase at even lower temperatures. Based on these results, we conclude that the high field regime indicated by the red color in Fig. 5 represents the helical superconducting state, and the low field regime by light blue corresponds to the BCS state. Although it is theoretically challenging to estimate quantitatively the momentum of Cooper pairs from experimental results, we can estimate the NRET values in the fluctuation regime near the upper critical field. The theoretical estimate54 of 10−17 Ωm3/A shows in good agreement with the experimentally observed 5 × 10−18 Ωm3/A. This strengthens the conclusion of our study.

The strong field-orientation dependence of intrinsic NRET likely appears as a result of the direction-dependent Doppler shift of the quasiparticles in d-wave superconductors. When H is applied parallel to the nodal direction, quasiparticles around the nodes perpendicular to the magnetic field are excited. When the current is applied parallel to these nodes, the system exhibits more metallic behavior compared with that for the antinodal direction. Although such a simple interpretation should be scrutinized, the present results also point toward the importance of nodal structure for the direction-dependent NRET. We note that the finite-momentum pairing state has been suggested in the pair-density-wave (PDW) state in the pseudogap phase of cuprates by scanning tunneling microscope measurements55. Therefore, it is highly intriguing to apply the present direction-dependent NRET to the putative PDW state.

The NRET effect arising from the intrinsic superconducting response observed in the tricolor d-wave superconducting superlattice with strong Rashba interaction provides evidence for the emergence of a superconducting state with finite-momentum Cooper pairs at high fields, most likely a helical superconducting state. Such a unique state provides a platform to investigate the novel fermionic superfluid systems beyond the BCS pairing states.

Methods

Device fabrication

The tricolor Kondo superlattices of YbCoIn5/CeCoIn5/YbRhIn5 were epitaxially grown on MgF2 substrates by the molecular beam epitaxy (MBE) technique. Firstly, a CeIn3 layer was grown as a buffer layer on the MgF2 substrate, then the 3-unit-cell-thick (3-UCT) YbCoIn5, 8-UCT CeCoIn5, and 3-UCT YbRhIn5 layers are alternatively stacked for 30 times. The total thickness of the superlattice is ~ 300 nm. The quality of the superlattices was checked by multiple techniques, including X-ray diffraction measurements. For detailed information on the sample growth and characterization, see Ref. (28). The superlattices were then patterned using the focused ion beam (FIB) technique (JEOL, JIB-4501). The current path was carefully aligned along [100], [110], [010], and [1\(\bar{1}\)0] directions. A Ga source was used to mill the sample. The width of the FIB-cut sample is ~ 20 μm. The standard silver paste was used to make electronic contacts.

Nonreciprocal transport

We measured the first and second harmonic resistance of superlattices by using an AC current source (Keithley, 6221) and AC lock-in amplifiers (Stanford Research Systems, SR830) in a dilution refrigerator. The current of 20 μA was applied to the sample. A frequency of 13.7 Hz was used. The dc-resistance was measured by the first harmonic resistance, Rdc = Rω. The Cernox thermometers with magnetic-field calibration were used to control the sample temperature. The in-plane magnetic field was precisely applied by using a built-in rotator. The sample temperature was carefully monitored so that the current did not heat the sample. The second harmonic resistance was antisymmetrized as a function of a magnetic field. To obtain the antisymmetrized component of R2ω from the raw data, we calculated \({R}_{2\omega }(H)=\frac{{R}_{2\omega }^{{{{{{{{\rm{raw}}}}}}}}}(H)-{R}_{2\omega }^{{{{{{{{\rm{raw}}}}}}}}}(-H)}{2}\).