μSR Study of Unconventional Pairing Symmetry in the Quasi-1D Na₂Cr₃As₃ Superconductor

Abstract

We report the finding of a novel pairing state in a newly discovered superconductor Na${}_2$Cr${}_3$As${}_3$. This material has a non-centrosymmetric quasi-one-dimensional crystal structure and is superconducting at $T_{\mathrm{C}}\sim$ 8.0 K. We find that the magnetic penetration depth data suggests the presence of a nodal line $p_z$-wave pairing state with zero magnetic moment using transverse-field muon-spin rotation (TF-$\mu$SR) measurements. The nodal gap observed in Na${}_2$Cr${}_3$As${}_3$ compound is consistent with that observed in isostructural (K,Cs)${}_2$Cr${}_3$As${}_3$ compounds using TF-$\mu$SR measurements. The observed pairing state is consistent with a three-band model spin-fluctuation calculation, which reveals the $S_z=0$ spin-triplet pairing state with the $sin{k}_z$ pairing symmetry. The long-sought search for chiral superconductivity with topological applications could be aided by such a novel triplet $S_z=0$ p-wave pairing state.

1. Introduction

The quest for spin-triplet superconductors in which Cooper pairs have finite angular momentum and equal spin, has been one of the significant research efforts notably due to its natural link to topologically related science and for possible unconventional superconductivity [1]. To date, the most promising systems for spin-triplet superconductivity are Uranium-based heavy-fermion compounds UTe${}_2$ [2], UGe${}_2$ [3], and UPt${}_3$ [4]. From the theoretical viewpoint [1], spin-triplet Cooper pairs are thought to originate directly from ferromagnetic (FM) fluctuations. Superconductivity in the vicinity of an antiferromagnetic (AFM) instability has been extensively explored in the last three decades or so [5] as in the case of high-temperature cuprates [6], iron pnictides [7], and heavy fermion systems [8]. Superconducting materials with a background of FM spin fluctuations are still rare, as observed A-phase of super-fluid ${}^3$He [9]. Sr${}_2$RuO${}_4$, and UPt${}_3$ are two promising candidates of chiral superconductors with plausible triplet p-wave and triplet f-wave pairing [10,11]. In a chiral superconductor, an angular momentum spontaneously develops and lowers its free energy by eliminating nodes in the gap.

In inorganic quasi one dimensional (Q1D) 3d-electron system, A${}_2$Cr${}_3$As${}_3$ (A = Na, K, Rb, and Cs), which crystallize in the non-centrosymmetric hexagonal structure with space group P-6m2 (No. 187) [12], it has been confirmed that the upper critical field $H_{\mathrm{c}2}$ perpendicular to Cr-chain is significantly larger than the Pauli limit, which strongly supports spin-triplet pairing [13]. Moreover, a nodal line gap symmetry was unveiled by magnetic penetration depth measurement on (K,Cs)${}_2$Cr${}_3$As${}_3$ [14,15,16] and Volovik-like field dependence of the zero-temperature Sommerfeld coefficients in the SC mixed state of A${}_2$Cr${}_3$As${}_3$ [17]. The spin-lattice relaxation rate (1/T${}_1$) of A${}_2$Cr${}_3$As${}_3$ decreases rapidly below $T_{\mathrm{C}}$ with no Hebel–Slichter peak and ubiquitously follows a $T^5$ variation below a characteristic temperature ∼0.6 $T_{\mathrm{C}}$, which indicates the existence of nodes in the superconducting gap function and ferromagnetic spin fluctuations within the sublattice of Cr atoms [18]. Neutron scattering measurements suggest subtle interplays of structure, electron-phonon, and magnetic interactions in K${}_2$Cr${}_3$As${}_3$ [19]. A recent, ${}^{75}$As nuclear quadrupole resonance study [18] suggests that the temperature dependence of the 1/T${}_1$, by changing A in the order of A = Na, Na${}_{0.75}$K${}_{0.25}$, K, and Rb, the system can be tuned to approach a possible FM QCP. The above properties of A${}_2$Cr${}_3$As${}_3$ suggest that these compounds are the possible solid-state analog of superfluid ${}^3$He. Hence, further investigations of these compounds are important to bridge three large research areas: strong correlations, unconventional superconductivity, and topological quantum phenomena.

In order to investigate the pairing mechanism and time reversal symmetry breaking in the ground state of novel superconductors, we have performed a systematic muon spin rotation and relaxation ($\mu$SR) study. Muon, a spin 1/2 subatomic particle, probed into the sample, precise around the local magnetic field, is a powerful tool to investigate superconducting materials [20]. In this paper, we have reported Na${}_2$Cr${}_3$As${}_3$ as a nodal gap superconductor with preserved time reversal symmetry as suggested by $\mu$SR measurement. Furthermore, our results are also supported by the electronic structure calculation. Electronic structure calculations reveal that owing to 1D nature of the crystal structure, the band structures feature weak in-plane dispersion and strong out-of-plane dispersion. The weak in-plane dispersion suffices to give a strong peak in the density-of-states, which is responsible for ferromagnetic fluctuations and spin-triplet superconductivity. There exists a quasi-three-dimensional Fermi surface (FS), and two quasi-one-dimensional FSs [21,22,23] which are strongly nested [13,24]. The FS nesting opens a spin-fluctuation pairing channel in both spin-singlet and triplet channels. We computed the SC pairing symmetry in a three-band Hubbard model. We report that the lowest-energy pairing state lies in a novel spin-triplet channel with total spin $S_z=0$, and the corresponding pairing symmetry is a $p_z=sin{k}_z$ like. This gives a nodal line gap and is also orbital selective. The results are found to be consistent with the experimental data.

2. Experimental Details

The powder sample of Na${}_2$Cr${}_3$As${}_3$ was prepared by the ion-exchange method with sodium naphthalene solution (Naph.-Na) in tetrahydrofuran (THF) using K${}_2$Cr${}_3$As${}_3$ powder as the precursor [25]. Transverse field muon spin rotation (TF-$\mu$SR) [26] measurements were carried out on the MUSR spectrometer at ISIS Neutron and Muon Facility, UK [27,28]. Small pieces (in pellet form) of Na${}_2$Cr${}_3$As${}_3$ were mounted in sealed titanium (99.99%) sample holder under He-exchange gas, which was placed in a He-3 system that has a temperature range of 0.3–11 K. Using an active compensation system, the stray magnetic fields at the sample position were canceled to a level of 1 $\mu$T. TF$-\mu$SR measurements were performed [29,30] in the superconducting mixed state in an applied field of 30 mT, well above the lower critical field of $H_{\mathrm{c}1}\sim$ 2 mT, but below the upper critical field of $H_{\mathrm{c}2}\sim$ 54 T of this material [31]. The TF$-\mu$SR data were collected in the field cooling mode, where the magnetic field 30 mT was applied at 11 K, above the superconducting transition $T_{\mathrm{C}}$, and the sample was then cooled down to 0.3 K. The data were analyzed using the open software package WiMDA [32].

3. Results and Discussion

3.1. Crystal Structure and Magnetization

The crystal structure of Na${}_2$Cr${}_3$As${}_3$ is shown in the left panel of Figure 1, which crystallizes in the hexagonal non-centrosymmetric structure with space group P-6m2 (No. 187), in which the (Cr${}_3$As${}_3$)${}^{2-}$ linear chains are separated by Na${}^{+}$ ions. Structurally, A${}_2$Cr${}_3$As${}_3$ have a typical Q1D configuration originated from the 1D CrAs chains that crystallize in a fashion of double-wall subnanotubes, with the alkali metal ions located among the interstitials of the CrAs chains [31]. The upper critical field ∼54 T exceed the Pauli paramagnetic limited = 1.84 $T_{\mathrm{C}}\sim$ 16 T [31], suggesting strongly coupled superconductivity in Na${}_2$Cr${}_3$As${}_3$, which is also observed previously in A${}_2$Cr${}_3$As${}_3$ (A = K, Rb, Cs) and ACr${}_3$As${}_3$ (A = K) superconductors [1]. Strong electron correlation effect is evident from large value of the Sommerfeld coefficient $\gamma$ as 76.5 mJ/(mol-K${}^2$) in Na${}_2$Cr${}_3$As${}_3$ [31], this is a common feature in A${}_2$Cr${}_3$As${}_3$ compounds due to reduced dimensionality [18]. In A${}_2$Cr${}_3$As${}_3$ series, $T_{\mathrm{C}}$ increases dramatically from 2.2 to 8.0 K from Cs${}^{+}$ to Na${}^{+}$ indicating substantial positive chemical pressure effect on $T_{\mathrm{C}}$ and interchain coupling [25].

3.2. TF-$\mu$SR Analysis

Previous theoretical and experimental studies of magnetic penetration depth using tunnel-diode oscillator, $\mu$SR and nuclear quadrupole resonance measurements confirm the presence of nodal gap in A${}_2$Cr${}_3$As${}_3$ (A = K, Rb, Cs) systems [13,14,15,16,18]. To understand the enigmatic superconducting gap structure of Na${}_2$Cr${}_3$As${}_3$, we have carried out the TF$-\mu$SR measurements. Figure 2a,b show the TF$-\mu$SR asymmetry-time spectra at 0.3 K (≪$T_{\mathrm{C}}$) and 9.0 K (>$T_{\mathrm{C}}$) obtained in FC mode with an applied field of 30 mT ($H>H_{c1}\sim$ 2 mT but below $H\ll H_{c2}\sim$ 54 T). The observed decay of the $\mu$SR signal with time below $T_{\mathrm{C}}$ is due to the inhomogeneous field distribution of the flux-line lattice. We have used an oscillatory decaying Gaussian function to fit the TF$-\mu$SR asymmetry spectra, which is given below [33,34],

$$G_{z1}\left(t\right)=A_{1}cos(2\pi {\nu }_{1}t+\theta )exp\left(\frac{-{\sigma }^2{t}^2}{2}\right)+A_{2}cos(2\pi {\nu }_{2}t+\theta )$$

(1)

where $A_1$, ${\nu }_1$ and are the asymmetry, frequency of the muon precession signal from the sample and $A_2$, ${\nu }_2$ are asymmetry and frequency of the background signal from the Ti-sample holder, respectively, while $\theta$ is the initial phase angle of the muon, with ${\gamma }_{\mu }/2\pi$ = 135.5 MHz T${}^{-1}$ is the muon gyromagnetic ratio. $A_2$ value is calculated from 0.3 K fitting data, $\theta$ values were kept zero. The total relaxation rate $\sigma$ contains two parts, superconducting vortex-lattice contributions (${\sigma }_{\mathrm{sc}}$) which is directly linked to the magnetic penetration depth ${\lambda }_{\mathrm{L}}$ and nuclear dipole moments (${\sigma }_{\mathrm{nm}}$). ${\sigma }_{\mathrm{nm}}\sim 0.17\mathsf{\mu }$s${}^{-1}$, is assumed to be constant over the entire temperature range between 0.3 K and 9 K, where $\sigma$ = $\sqrt{({\sigma }_{\mathrm{sc}}^2+{\sigma }_{\mathrm{nm}}^2)}$. ${\sigma }_{\mathrm{nm}}$ is determined by fitting TF$-\mu$SR above $T_{\mathrm{C}}$. The red lines in Figure 2a,b illustrate the fits of the TF$-\mu$SR data. The parameter $A_2$ was kept fixed in the fitting between 0.3 K and 9 K. $T_{\mathrm{C}}$ derived from ${\sigma }_{\mathrm{sc}}$ data is ∼8.0 K as shown in Figure 2c.

The magnetic penetration depth ${\lambda }_{\mathrm{L}}$ is related to ${\sigma }_{\mathrm{sc}}$ by the expression [35,36], ${\sigma }_{\mathrm{sc}}^2/{\gamma }_{\mu }=0.00371{\Phi }_0^2/{\lambda }_{\mathrm{L}}^4$, where ${\Phi }_0$ = 2.068 × 10${}^{-15}$ Wb is the magnetic-flux quantum. ${\lambda }_{\mathrm{L}}\left(T\right)$ is related to the superfluid density and can be used to determine the nature of the superconducting gap. The temperature dependence of ${\sigma }_{\mathrm{sc}}\left(T\right)$ is shown in Figure 2c. Below 1 K, it increases in a linear fashion. This non-constant low temperature behavior is a hallmark of superconducting gap nodes. By analyzing the superfluid density data with different models of the gap function ${\Delta }_k\left(T\right)$, the pairing symmetry of Na${}_2$Cr${}_3$As${}_3$ can be understood. We calculate the superfluid density for a given pairing model as follows [37,38]:

$$\begin{array}{ccc}\hfill \frac{{\sigma }_{\mathrm{sc}}\left(T\right)}{{\sigma }_{\mathrm{sc}}\left(0\right)}& =& \frac{{\lambda }_{\mathrm{L}}^{-2}\left(T\right)}{{\lambda }_{\mathrm{L}}^{-2}\left(0\right)}\hfill \\ \hfill & =& 1+2{〈{\int }_{{\Delta }_k\left(T\right)}^{\infty }\frac{E}{\sqrt{E^2-{\left|{\Delta }_k\left(T\right)\right|}^2}}\frac{\partial f}{\partial E}dE〉}_{\mathrm{FS}}\hfill \end{array}$$

(2)

where $f={[1+exp\left(\frac{E}{k_{B}T}\right)]}^{-1}$ is the Fermi function and ${\langle \rangle }_{\mathrm{FS}}$ represents the Fermi surface’s average (assumed to be spherical). We take ${\Delta }_k\left(T\right)=\Delta \left(T\right){\mathrm{g}}_k$, where we assume a temperature dependence that is universal $\Delta \left(T\right)={\Delta }_{0}tanh\left[1.82{\left\{1.018(T_{\mathrm{C}}/T-1)\right\}}^{0.51}\right]$. The magnitude of the gap at 0 K is ${\Delta }_0$, and the function ${\mathrm{g}}_k$ denotes the gap’s angular dependence [37,38] and is given for the various models in

Table 1. A summary of the different gap symmetries were used to fit the magnetic penetration depth in Figure 2 for Na${}_2$Cr${}_3$As${}_3$ with $T_{\mathrm{C}}\sim$ 8.0 K. The first column corresponds to the models in the figure, g${}_k$ gives the angular dependence of the gap and 2$\Delta \left(0\right)$/k${}_{\mathrm{B}}{T}_{\mathrm{C}}$ is the gap magnitude in the calculation that best fitted the data.

Pairing State	g${}_{\mathit{k}}$	Gap $\mathbf{\Delta }\left(0\right)$(meV)	2$\mathbf{\Delta }\left(0\right)$/k${}_{\mathbf{B}}{\mathit{T}}_{\mathbf{C}}$
s-wave	1	1.45(2)	4.21
p-wave (point)	$sin\theta$	1.80(3)	5.22
p-wave (line)	$cos\theta$	3.15(6)	9.14

[39,40].

We have analyzed the temperature dependence of ${\sigma }_{\mathrm{sc}}$ based on different models (isotropic s-wave, p-wave line node, and p-wave point node) as shown in Figure 2c. The fit to ${\sigma }_{\mathrm{sc}}\left(T\right)$ data of Na${}_2$Cr${}_3$As${}_3$ gives 2$\Delta \left(0\right)$/$k_{\mathrm{B}}{T}_{\mathrm{C}}$ = 4.21 for a single isotropic s-wave, 2$\Delta \left(0\right)$/$k_{\mathrm{B}}{T}_{\mathrm{C}}$ = 5.22 for a p-wave point node, and 2$\Delta \left(0\right)$/$k_{\mathrm{B}}{T}_{\mathrm{C}}$ = 9.14 for a p-wave line node. It is clear from Figure 2c that the isotropic s-wave or p-wave point gap does not fit the data. On the other hand, p-wave line node best fits ${\sigma }_{sc}\left(T\right)$ data. So this result confirms unconventional pairing mechanism in Na${}_2$Cr${}_3$As${}_3$. The observed 2$\Delta \left(0\right)$/$k_{\mathrm{B}}{T}_{\mathrm{C}}$ values are consistent with those found in other compounds in this family [15]. The TF-$\mu$SR data suggest the presence of line nodes in the superconducting energy gap. The TF-$\mu$SR results of (K,Cs)${}_2$Cr${}_3$As${}_3$ [15], also support the presence of line nodes in the superconducting gap.

Furthermore, the large gap value obtained from the nodal p-wave fit is much larger than the gap value expected for BCS superconductors (3.53), indicating the presence of strong coupling superconductivity, which is in line with the observed gap values found in (K,Cs)${}_2$Cr${}_3$As${}_3$ [15]. The observed gap symmetry in Na${}_2$Cr${}_3$As${}_3$ together with ${}^{75}$As nuclear quadrupole resonance and theoretical calculations [18] in A${}_2$Cr${}_3$As${}_3$ suggest unconventional pairing mechanism in (Na,K,Rb,Cs)${}_2$Cr${}_3$As${}_3$. A summary of the different gap symmetries were used to fit the magnetic penetration depth for Na${}_2$Cr${}_3$As${}_3$ is shown in Table 1. Furthermore, from our TF-$\mu$SR data we have estimated the magnetic penetration depth ${\lambda }_{\mathrm{L}}\left(0\right)$, superconducting carrier density $n_{\mathrm{s}}$ [${\lambda }_{\mathrm{L}}^2=m^{\ast }{c}^2/4\pi n_s{e}^2$], and effective-mass enhancement $m^{\ast }$ [$m^{\ast }=(1+{\lambda }_{el-ph})m_e$ where ${\lambda }_{el-ph}$ is the electron phonon coupling strength] to be ${\lambda }_{\mathrm{L}}\left(0\right)$ = 790(4) nm (from the nodal p-wave fit), $n_{\mathrm{s}}$ = 8.5(1) × 10${}^{26}$ carriers/m${}^3$, and $m^{\ast }$ = 1.884(3) $m_{\mathrm{e}}$, respectively. A${}_2$Cr${}_3$As${}_3$ family is known for having a large magnetic penetration depth [15]. This is due to the strong interaction that occurs as a result of the quasi-one-dimensional structure. For K${}_2$Cr${}_3$As${}_3$, ${\lambda }_{\mathrm{L}}\left(0\right)$ = 646(3) nm, Cs${}_2$Cr${}_3$As${}_3$, ${\lambda }_{\mathrm{L}}\left(0\right)$ = 954(2) nm [15].

3.3. Zero Field MuSR

ZF$-\mu$SR were used to check for the presence of any hidden magnetic ordering in Na${}_2$Cr${}_3$As${}_3$. Figure 3 compares the zero field time-dependent asymmetry spectra above and below and $T_{\mathrm{C}}$ (for T = 0.28 K and 10.0 K). The ZF$-\mu$SR data can be well described using a damped Gaussian Kubo–Toyabe (KT) function [41],

$$G_{\mathrm{z}2}\left(t\right)=A_3{G}_{\mathrm{KT}}\left(t\right)e^{-{\lambda }_{\mu }t}+A_{\mathrm{bg}},$$

(3)

where $G_{\mathrm{KT}}\left(t\right)=[\frac{1}{3}+\frac{2}{3}(1-{\sigma }_{\mathrm{KT}}^2{t}^2)exp\left(-\frac{{\sigma }_{\mathrm{KT}}^2{t}^2}{2}\right)]$, is known as the Gaussian Kubo–Toyabe function, $A_3$ is the zero field asymmetry of the sample signal, $A_{\mathrm{bg}}$ is the background signal, ${\sigma }_{\mathrm{KT}}$ and ${\lambda }_{\mu }$ represents the electronic relaxation rate (the local field distribution width $H_{\mu }=\sigma /{\gamma }_{\mu }$). No sign of muon spin precession is visible either at 0.28 K or 10 K, ruling out the presence of large internal field as seen in magnetically ordered systems. The only possibility is that the muon spin relaxation is due to static, randomly oriented local fields associated with the electronic and nuclear moments at the muon site. As shown in Figure 3 both the ZF-asymmetry spectra fall on top of each other, which confirms the absence of spontaneous magnetic field due to time reversal symmetry breaking in case of Na${}_2$Cr${}_3$As${}_3$.

Fits to the ZF$-\mu$SR asymmetry data using Equation (3) and shown by the solid lines in Figure 3 give ${\sigma }_{\mathrm{KT}}=0.094\mathsf{\mu }{\mathrm{s}}^{-1}$ and ${\lambda }_{\mu }=0.057\mathsf{\mu }{\mathrm{s}}^{-1}$ at 10 K and ${\sigma }_{\mathrm{KT}}=0.098\mathsf{\mu }{\mathrm{s}}^{-1}$ and ${\lambda }_{\mu }=0.053\mathsf{\mu }{\mathrm{s}}^{-1}$ at 0.28 K.

4. Theoretical Calculations

Earlier electronic structure calculations have shown that the low-energy properties are defined by a minimal three-band model, stemming mainly from the $d_{z^2}$, $d_{xy}$, and $d_{x^2-y^2}$ orbitals of the Cr-atoms [13,42,43,44]. We adopt the three-band tight-binding model from Ref. [13] and the theoretical details are given in the Appendix A. The corresponding Fermi surfaces (FSs) are shown in Figure 4a, with a gradient color denoting the corresponding orbital weight. Interestingly, there lie two flat FS sheets at constant $k_z$ cuts which have weak basal plane anisotropy. Such FSs govern strong peaks in the density of state (DOS) at the Fermi level, and hence ferromagnetic fluctuations. In addition, due to the separation of the flat FS sheets between the nearly constant $\pm k_z^{\ast }$ direction, there arises strong FS nestings around $\mathbf{Q}\to (0,0,Q_z)$, where $Q_z=2k_z^{\ast }$. Such a nesting promotes magnetic fluctuation mediated pairing channel which follows the relation $\mathrm{sgn}\left[{\Delta }_{\mathbf{k}}\right]=-\mathrm{sgn}\left[{\Delta }_{\mathbf{k}+\mathbf{Q}}\right]$. Through numerical calculation, we show below that the pairing symmetry turns out to be $p_z$ in nature with triplet pairing channel but for $S=0$. We notice that the FS topology of this material is qualitatively similar to the iso-structural heavy-fermion superconductor UPt${}_3$ [45,46] in which also unconventional p-wave pairing symmetry due to FM fluctuation has been discussed before [46,47].

We compute the pairing state ${\Delta }_{\mathbf{k}}$ as the eigenfunction of the leading eigenvalue of the spin-fluctuation mediated pairing interaction ${\tilde{\Gamma }}_{\uparrow \uparrow }(\mathbf{k}-{\mathbf{k}}^{\prime })$ by solving the following equation:

$$\begin{array}{c}\hfill \Delta \left(\mathbf{k}\right)=-\lambda \frac{1}{{\Omega }_{\mathrm{BZ}}}\sum _{{\mathbf{k}}^{\prime }}{\Gamma }_{\uparrow \downarrow }(\mathbf{k}-{\mathbf{k}}^{\prime })\Delta \left({\mathbf{k}}^{\prime }\right).\end{array}$$

(4)

${\Omega }_{\mathrm{BZ}}$ denote the Brillouin zone volume. $\lambda$ is the pairing eigenvalue (proportional to the SC coupling strength), and $\Delta \left(\mathbf{k}\right)$ is the corresponding pairing eigenfunction. For the calculation of ${\tilde{\Gamma }}_{\uparrow \uparrow }(\mathbf{k}-{\mathbf{k}}^{\prime })$, we consider a three-band Hubbard model with intra-, inter-orbital Hubbard interactions, Hund’s coupling, and pair-hopping terms. Then, we obtain the pairing potential by considering the bubble and ladder diagrams [48,49,50,51,52,53]:

$$\begin{array}{ccc}\hfill {\tilde{\Gamma }}_{\uparrow \downarrow }\left(\mathbf{q}\right)& =& \frac{1}{2}\left[3{\tilde{U}}_s{\tilde{\chi }}_s\left(\mathbf{q}\right){\tilde{U}}_s-{\tilde{U}}_c{\tilde{\chi }}_c\left(\mathbf{q}\right){\tilde{U}}_c+{\tilde{U}}_s+{\tilde{U}}_c\right].\hfill \end{array}$$

(5)

Here we only present the results for the spin-flip component of the pairing potential, while the pairing with finite spin components (${\tilde{\Gamma }}_{\uparrow \uparrow }/{\tilde{\Gamma }}_{\downarrow \downarrow }$) are also considered but found to be much lower in strength. This is consistent with the absence of a finite magnetic moment in the muon experimental data. The symbol ‘tilde’ denotes a tensor in the orbital basis. The subscripts ‘s’ and ‘c’ denote spin and charge density-density fluctuation channels, respectively. ${\tilde{\chi }}_{s/c}$ are the spin and charge density–density correlation functions (tensors in the same orbital basis), computed within the random-phase-approximation (RPA). ${\tilde{U}}_{s/c}$ are the on-site interaction tensors for spin and charge fluctuations, respectively, whose non-vanishing components are the non-zero components of the matrices ${\tilde{U}}_c$ and ${\tilde{U}}_s$ are given as [54]: ${\left({\tilde{U}}_{s,c}\right)}_{\alpha \alpha }^{\alpha \alpha }=U_{\alpha }$, ${\left({\tilde{U}}_s\right)}_{\beta \beta }^{\alpha \alpha }=\frac{1}{2}{J}_H$, ${\left({\tilde{U}}_c\right)}_{\beta \beta }^{\alpha \alpha }=2V-J_H$, ${\left({\tilde{U}}_s\right)}_{\alpha \beta }^{\alpha \beta }=V$, ${\left({\tilde{U}}_c\right)}_{\alpha \beta }^{\alpha \beta }=-V+3J_H$, ${\left({\tilde{U}}_{s,c}\right)}_{\alpha \beta }^{\beta \alpha }=J^{\prime }$. $\alpha$, $\beta$ are orbital indices. The intra-orbital Hubbard interaction for the three orbitals are $U_m$ = 400, 200, 200 meV, the inter-orbital interaction is V = 150 meV, and Hund’s coupling and pair-hopping interactions are $J_H=J^{\prime }$ = 50 meV. These values are deduced from the Kanamori criterion and the pairing eigenfunctions do not change with the parameter values, while the pairing interaction increases with increasing interactions.

The interplay between FS topology, nesting, and pairing symmetry can be understood as follows. For repulsive interaction and $\lambda >0$ in Equation (4), the pairing eigenstate $\Delta \left(\mathbf{k}\right)$ must change sign over the FS to compensate for the negative sign in the left hand side of Equation (4). $\Delta \left(\mathbf{k}\right)$ changes sign between $\mathbf{k}$ and ${\mathbf{k}}^{\prime }$ which may be in a given band or between different bands. These two momenta are connected by the nesting feature at $\mathbf{q}=\mathbf{k}-{\mathbf{k}}^{\prime }$ at which ${\Gamma }_{\uparrow /\downarrow }\left(\mathbf{q}\right)$ acquires strong peaks. The locii of the peaks in ${\Gamma }_{\nu {\nu }^{\prime }}^{\prime }\left(\mathbf{q}\right)$ is primarily dictated by the FS nesting, while the overall amplitude is determined by the interaction strength.

We solve Equation (4) for the three FSs plotted on in Figure 4a. Our direct eigenvalue and eigenfunction solver yields the higher eigenvalue to be $\lambda \sim$0.1 and the corresponding eigenfunction gives a $p_z=sin\left(k_z\right)$ symmetry. We plot the eigenfunction as a color gradient map on several representative FS cuts in Figure 4c. We find that the gap $\Delta \left(\mathbf{k}\right)$ is odd under the Mirror symmetry along the $k_z$-direction, and changes sign between $\pm k_z$. There is a slight in-plane anisotropy on the gap, but not significant enough to promote sign-reversal in the $k_x$, $k_y$ plane. This particular pairing symmetry is consistent with the nesting properties between the two flat FS sheets across $\pm k_z^{\ast }$ as discussed above. The same pairing state is obtained in previous calculations in this family of materials and is also obtained in UPt${}_3$ superconductor [13,42].

The $p_z$ pairing symmetry being odd in parity is consistent with a spin-triplet Cooper pair. Among the three spin-triplet channels, the spin-flip term $1/\sqrt{2}(\uparrow \downarrow +\downarrow \uparrow )$ does not induce any spin-polarization. This is also the pairing channel we find to be dominant compared to the spin-polarized channels. Therefore, despite the time-reversal symmetry breaking, this state does not induce any magnetic moment, and thus the time-reversal breaking is not detectable in the muon experiment. This result is consistent with our zero-field $\mu$SR on Na${}_2$Cr${}_3$As${}_3$ measurements.

The obtained $p_z$ pairing channel gives a nodal line gap on the $k_z=0$ FS cut, as shown in the middle plot in Figure 4c. The corresponding nodal structure appears in a ‘V’ shape DOS shown in Figure 4b by the blue line. We also split the contributions to the DOS from three different orbitals, as shown in different colors. We notice that since the FS near the $k_z=0$ region is dominated by mainly the $d_{x^2-y^2}$ orbital, the nodal structure is mainly obtained in this orbital, while the other two orbitals see very much fully gapped behavior. Given that the total DOS has a ‘V’-shave behavior, the low-temperature dependence of the superfluid density acquires a linear-in-T dependence as seen experimentally.

5. Conclusions

In summary, we have presented TF-$\mu$SR result in the superconducting state of Na${}_2$Cr${}_3$As${}_3$, which has a Q1D non-centrosymmetric crystal structure. The temperature dependence of magnetic penetration depth obtained from the TF-$\mu$SR results confirm the presence of p-wave line node in the superconducting gap structure. Despite a p-wave, triplet pairing state, we do not find any evidence of a magnetic moment of the Cooper pair. These results are consistent with the theoretical calculation. The theory is developed for a three-band Hubbard model and the pairing potential is obtained through many-body effects. We find that the lowest energy state of superconductivity is a spin-triplet p-wave, but in the $S_z=0$ channel. The corresponding pairing state possesses a $p_z$ symmetry which changes sign across the $k_z=0$ mirror plane and stems from the FS nesting between quasi-flat FS sheets lying at some $\pm k_z$ planes. Such a spin-zero triplet p-wave pairing channel is a novel pairing state which can be potentially important for chiral superconductivity and topological phases.