## Abstract

When a theoretical model is realized in nature, small perturbation terms play important roles in the selection of the ground state in geometrically frustrated magnets. In case of a triangular spin tube, the two-dimensional network of the inter-tube interaction forms characteristic lattices. Among them Kagome-Triangular (KT) lattice is known to exhibit an enriched phase diagram including various types of non-trivial structures: non-coplanar cuboc structure, coplanar 120° structure with the two-dimensional propagation vector of \({\boldsymbol{k}}_{2\mathrm{D}}\) = (0, 0), \(\sqrt 3 \times \sqrt 3\) structure with \({\boldsymbol{k}}_{2{\mathrm{D}}}\) = (1/3, 1/3), and incommensurate structure. We investigate the magnetic state in the model material CsCrF_{4} by using neutron diffraction technique. Combination of representation analysis and Rietveld refinement reveals that a very rare structure, i.e., a quasi-120° structure with \({\boldsymbol{k}}_{2{\mathrm{D}}}\) = (1/2, 0), is realized at the base temperature. The classical calculation of the phase diagram elucidates that CsCrF_{4} is the first experimental realization of the KT lattice having ferromagnetic Kagome bond. A single-ion anisotropy and Dzyaloshinskii-Moriya interaction play key roles in the selection of the ground state. Furthermore, a successive phase transition having an intermediate state represented by \({\boldsymbol{k}}_{2{\mathrm{D}}}\) = (1/3, 1/3) is observed. The intermediate state is a partially ordered 120° structure which is induced by thermal fluctuation.

## Introduction

Geometrical frustration in a magnetic material prevents the conventional Néel order and induces a non-trivial magnetic state at low temperatures. Particularly the two-dimensional (2D) triangular lattice has been extensively studied since the pioneering work on the quantum spin liquid in the Heisenberg antiferromagnet.^{1} A consensus is that the ground state is the ordered state with 120° structure but is very close to quantum criticality.^{2,3} In real compounds additional terms or perturbations such as anisotropy, further neighbor interaction, lattice distortion, etc., lift the macroscopic degeneracy of the ground state, and they lead to a variety of magnetic states.^{4,5,6,7,8} Drastic changes caused by small perturbations in highly degenerated systems have attracted a lot of attention in condensed matter physics.

In one-dimensional (1D) systems quantum fluctuation as well as geometrical frustration induces non-trivial magnetic states. One of the examples is a frustrated triangular spin tube, where antiferromagnetic spins on triangular vertices are arrayed in one dimension. An early work on Heisenberg *S* = 1/2 spin tube reveals that the ground state is a dimerized non-magnetic state having a unit of a two-site rung singlet.^{9} A finite energy gap in the magnetic dispersion and the exponential decay in spin correlation are predicted, and many theoretical studies have been reported so far.^{10,11,12,13,14,15,16} Similar to the 2D systems, a small perturbation induces drastic change in the ground state.^{17} Lattice distortion in the triangular rung breaks *Z*_{2} symmetry, suppresses the spin gap, and induces a Tomonaga-Luttinger Liquid (TLL) state with vector chiral order.^{18,19} In the classical Heisenberg system, on the other hand, a 120° structure is the ground state.

When the triangular spin tube is realized in nature, a geometry of the inter-tube interactions plays important roles. Particularly in the absences of frustration along the leg direction, the 2D-spin Hamiltonian in the plane perpendicular to the leg determines the spin structure. As an example of the tube configurations, supertriangular lattice in triangular lattice is shown in Fig. 1a. Here the triangular plaquettes are the cross sections of the tubes. The number of inter-triangular interactions of the lattice indicated by the red lines in Fig. 1a is four, which is the same as the coordination number in kagome lattice. In fact this supertriangular lattice can be transformed to Kagome-Triangular (KT) lattice^{20} by reducing the length of the red lines as shown in Fig. 1b. Here nearest neighbor bond is *J*_{2}, which we will call *main Kagome bond* or simply *Kagome bond* hereafter, and the next-nearest neighbor (NNN) bond is *J*_{1}, which we will call *Triangular bond*. It is noted that two of four NNN interactions in the kagome lattice are effective. The lattice exhibits various phases in the *J*_{1}−*J*_{2} phase diagram as shown in Fig. 1c. The signs of *J*_{i}s are positive for antiferromagnetic (AF) and negative for ferromagnetic (F), and the interaction is isotropic Heisenberg type. The predicted structures are non-coplanar cuboc, coplanar 120° with *k*_{2D} = (0, 0), that with *k*_{2D} = (1/3, 1/3), and incommensurate structures. Here the cuboc structure in the region of F-*J*_{2} and AF-*J*_{1} is a multi- *Q* structure having a 12-sublattice with the spins directing along the 12-middle points of a cube.^{20,21,22} As far as we know, the reported magnetic structures of Kagome magnets in the absence of lattice distortion are threefold: (i) the 120° structure with *k*_{2D} = (0, 0) in Fe and Cr-Jarosites,^{23,24,25,26,27,28} the semimetals Mn_{3}Sn, Mn_{3}Ge,^{29} and rare-earth tripod kagome,^{30} (ii) the \(\sqrt 3 \times \sqrt 3\) structure with *k*_{2D} = (1/3, 1/3) in high pressure phase in herbersmithite ZnCu_{3}(OH)_{6}Cl_{2},^{31} and (iii) the inplane ferromagnetic structure in V-Jarosite.^{32} A material having F-*J*_{2} and AF-*J*_{1} which would exhibit non-trivial magnetic states has not been reported so far.

The rare experimental realization of the equilateral triangular spin tube having the KT geometry is CsCrF_{4}.^{33} The crystal structure is shown in Figs. 1d, e. Cr^{3+} (3*d*^{3}) ions, which are Jahn-Teller inactive and carry Heisenberg spins, form an equilateral triangular tube along the crystallographic *c* direction. The space group is *P*6̄2*m* with a hexagonal structure, and the lattice is free from distortion down to low temperatures. In the CrF_{6} octahedron, the quasi-square of F_{4} in the *ab* plane is slightly distorted to an isosceles trapezoid. The main origin of the magnetic interaction between Cr^{3+} ions is a super exchange interaction via F^{−} ion. The angles of Cr-F-Cr for the rung direction is 148° and that for the chain direction is 180°, which indicate that both of the interaction along the leg *J*_{0} and that along the rung *J*_{1} are antiferromagnetic. The inter-tube interaction *J*_{2} in the *ab* plane, which corresponds to the Kagome bond, is depicted by the dotted lines in Fig. 1e. The geometry is the same as that in Fig. 1a, meaning that the spin lattice is equivalent to the non-distorted KT lattice in Fig. 1b.^{22}

The magnetic susceptibility of CsCrF_{4} showed a broad maximum at *T* ~ 60 K, suggesting development of a short-range antiferromagnetic spin correlation.^{34,35} Heat capacity showed no lambda-type anomaly above *T* = 1.5 K, and no clear evidence for a phase transition has been detected. The magnetic state was originally discussed in the context of the isolated spin tube. The heat capacity showed, however, a small bending around *T* = 3 K. Furthermore, a slight hysteresis was observed in the magnetic susceptibility between Zero Field Cooling (ZFC) and Field Cooling (FC) processes below *T* = 5 K. Broad peaks were observed for the linear and non-linear components of the AC susceptibility at 4 K and 3 K, respectively.^{36} The details of the magnetic state of CsCrF_{4} at low temperatures are, thus, complicated and unclear, and the frustrated two-dimensional geometry may have an important role.

In this paper, we demonstrate that non-trivial magnetic long-range ordered states are induced in CsCrF_{4} which is a model compound of the KT lattice having the ferromagnetic Kagome bond by using neutron diffraction technique. Combination of the magnetic structure analysis and the calculation of the phase diagram reveals that a single-ion anisotropy and DM interaction select a very rare magnetic structure, i.e., quasi-120° structure with *k*_{2D} = (1/2, 0), at the base temperature. Furthermore, a successive phase transition is observed, and the intermediate temperature phase is partially ordered 120° structure.

## Results

### Neutron diffraction

The neutron diffraction profiles at 10 K in Fig. 2a is reasonably reproduced by the calculation based on the crystal structure of CsCrF_{4} previously reported in ref. ^{33}. The refined lattice parameters and atomic positions are summarized in Supplementary Note 2. As shown in Fig. 2b a broad peak is observed at 2*θ* ~ 25°, which corresponds to *Q* ~ 1.2 Å, at 10 K. The temperature is much lower than the maximum temperature (60 K) of the bulk susceptibility,^{35} and the broad peak is ascribed to the development of magnetic short-range correlation. At 100 K, in contrast, the broad peaks is suppressed, and paramagnetic diffuse scattering exists in the small 2*θ*.

Figure 3a shows the diffraction profile obtained by subtracting the data at 10 K from that at 1.6 K. The details of the background subtraction are described in Supplementary Note 3. Well-defined peaks are observed, meaning that a magnetic order is realized. A spin liquid state that was originally supposed as the ground state^{34,35} is, thus, not the case in CsCrF_{4}. Two-dimensional geometry of the inter-tube interaction is more important than the quantum nature of one-dimensional spin tube. We, hence, found that CsCrF_{4} is an ideal model for the non-distorted KT lattice, where the main Kagome bond *J*_{2} would be smaller than the Triangular bond *J*_{1}. The magnetic Bragg peaks are all indexed by (*h k l*) with *h* = half integer, *k* = integer, and *l* = half integer. The propagation vector is identified as \({\boldsymbol{k}}_1 = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\) which coincides with the cuboc structure predicted in the KT lattice. This suggests that CsCrF_{4} is a very rare experimental realization of the KT lattice having ferromagnetic Kagome bond. Figure 3b shows the subtracted profile measured at 3.0 K. The 2*θ*s of the magnetic peaks are different from those measured at 1.6 K. The magnetic propagation vector is identified as \({\boldsymbol{k}}_2 = \left( {\frac{1}{3},\frac{1}{3},\frac{1}{2}} \right)\). The *k*_{1} and *k*_{2} coincide with high symmetry points in the first Brillouin zone, L and H in Fig. 1f, respectively.

The temperature evolution of the neutron profile without background subtraction in a heating process is shown in Fig. 3c. The variation of the 2*θ* positions of the magnetic peaks means a successive transition. Temperature dependences of the intensities of the magnetic Bragg peaks at \(\left( {\frac{1}{2}\bar 1\frac{1}{2}} \right)\) and \(\left( {\frac{2}{3}\frac{2}{3}\frac{1}{2}} \right)\) are shown in Fig. 4a. The peak at \(\left( {\frac{1}{2}\bar 1\frac{1}{2}} \right)\) disappears at about *T*_{N1} = 2.8 K. We define the ordered phase at *T* ≤ *T*_{N1} as the low temperature (LT) phase. At *T* ≥ *T*_{N1} the peak at \(\left( {\frac{2}{3}\frac{2}{3}\frac{1}{2}} \right)\) disappears at about *T*_{N2} = 3.5 K. We define the ordered phase at *T*_{N1} ≤ *T* ≤ *T*_{N2} as the intermediate temperature (IT) phase. The diffuse scattering is suppressed below *T*_{N1} but still remains even at 1.6 K, which can be seen in Fig. 3c as well as Fig. 2b. The temperature dependences of the full width at half maximum (FWHM) of the peak of \(\left( {\frac{1}{2}2\frac{1}{2}} \right)\) at 2θ = 43.7° and \(\left( {\frac{4}{3}\frac{1}{3}\frac{1}{2}} \right)\) at 2*θ* = 31.7° are shown in Fig. 4b. The gray area is the experimental resolution estimated from the nuclear peak of (0 0 1) at 10 K. The dashed line is the FWHM of the peak, and the dotted lines are the errors for the FWHM. The FWHM of the peak at \(\left( {\frac{4}{3}\frac{1}{3}\frac{1}{2}} \right)\) in the IT phase is wider than the resolution, meaning that the magnetic order in the IT phase is not truly long-ranged. The FWHMs at \(\left( {\frac{1}{2}2\frac{1}{2}} \right)\) in the LT phase are much narrower than those in the IT phase, and they are resolution limited. Slight broadening at 2.4 K is ascribed to the uncertainty of the fitting. From the difference between the FWHM of the magnetic peak and the experimental resolution, the correlation length of the spins is estimated as a function of the temperature as shown in Fig. 4c. The maximum limit of the correlation length indicated by the dashed line is estimated as 800 Å. The correlation length gradually increases with the decrease of the temperature at *T*_{N1} ≤ *T* ≤ *T*_{N2}, and it is beyond the maximum limit at *T* ≤ *T*_{N1}. The details of the estimate of FWHM and correlation length are described in Supplementary Notes 4 and 5, respectively.

### Magnetic structure analysis

The propagation vector of the LT phase is \({\boldsymbol{k}}_1 = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\), and the scaler of the *k*_{1} coincides with that of the propagation vectors of the triple-*k* cuboc structure, \({\boldsymbol{k}}_1^1 = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\), \({\boldsymbol{k}}_1^2 = \left( {0, - \frac{1}{2},\frac{1}{2}} \right)\), and \({\boldsymbol{k}}_1^3 = \left( { - \frac{1}{2},\frac{1}{2},\frac{1}{2}} \right)\). Since the cuboc structure is predicted in Heisenberg KT lattice,^{20} we simulate the neutron diffraction profile as shown in Fig. 2c. The calculated intensity at \({\boldsymbol{q}} = \left( {\frac{1}{2}\bar 1\frac{1}{2}} \right)\) which corresponds to 2*θ* = 23.5° is zero. In contrast, the magnetic peak is clearly observed. This means that the cuboc structure is not realized in CsCrF_{4}, suggesting that some additional perturbation terms are necessary. The detail of the cuboc structure is described in the Supplementary Note 6.

Next we construct spin models of single ** k** structures. Irreducible representations (IRs) and their basis vectors that satisfy the space group

*P*6̄2

*m*and the propagation vector \({\boldsymbol{k}}_1 = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\) are listed in Table 1. Because

*k*_{1}breaks three-fold rotational symmetry of the hexagonal system, all the three Cr sites are not equivalent; the A and B sites are equivalent, but the C site is inequivalent. We assume that the magnetic structure in the LT phase is associated to a single IR.

^{37}We also assume that the magnitude of the moments on the Cr ions are the same. The candidates of the magnetic structures are, then, linear combinations of

*ψ*

_{2},

*ψ*

_{3}, and

*ψ*

_{7}for Γ

_{2}, those of

*ψ*

_{4}and

*ψ*

_{8}for Γ

_{3}, and those of

*ψ*

_{5},

*ψ*

_{6}, and

*ψ*

_{9}for Γ

_{4}. In order to consider a high-symmetry structure, we first pick up 14 structures where the angles between the neighboring spins are fixed as 0°, 60°, 120° and 180° as listed in Table 2. The magnetic moments are expressed as follows;

Rietveld analyses were performed on the models A_{1}–A_{14}, and the results are presented. The parameters of the crystal structure are fixed to those at 10 K. Furthermore, the angles between the spins are fixed, meaning that the ratios among *C*_{i} are fixed, and the number of the free parameters in the refinement is one. The reasonable agreement to the data was obtained for four 120° structures; A_{2}, A_{5}, A_{10} and A_{14}. To distinguish these 120° structures, we define vector chirality ** κ** as follows;

where *i*, *j* and *k* are assigned A, B or C, *ε*_{ijk} means Levi-Civita symbol, and \(\widehat {\boldsymbol{m}}{\kern 1pt} _i\) is a magnetic moment normalized to 1. For the A_{2} and A_{10} models *κ*_{c} = 1, and for the A_{5} and A_{14} models *κ*_{c} = −1. Here *κ*_{c} is the *c* component of ** κ**. Next, we release the constraint of the angles between the neighboring spins, and we refined the coefficients of basis vectors for these four models. The results and the obtained models B

_{1}–B

_{4}are shown in the lower panel in Table 2. The fitting indexes

*χ*

^{2}and

*R*

_{wp}are improved, and among the models the B

_{1}and B

_{4}are better. For example the fitting curve for the model B

_{1}is indicated by the solid black curve in Fig. 3a. The fit to the data is good.

*ξ*,

*ζ*, and

*η*in Table 2 are the angles of the moments on A and B sites, B and C sites, and C and A sites, respectively. We found that the models B

_{1}in Fig. 5a and B

_{4}in Fig. 5b, both of which are quasi-120° structures, are the final candidates of the magnetic structure in the LT phase in CsCrF

_{4}. The moment sizes are about 1.4~1.5

*μ*

_{B}for both candidates and they are considerably smaller than 3

*μ*

_{B}, the full moment of Cr

^{3+}ion. They are strongly fluctuated due to the geometrical frustration and the low dimensionality of the system. The details of the model fitting is described in Supplementary Note 3.

For the IT phase, due to broad widths of the magnetic Bragg peaks and large diffuse scattering, the peak profile could not be refined very accurately. Nevertheless, we performed Rietveld fit to the subtracted profile at 3 K on the basis of two models. One is \(\sqrt 3 \times \sqrt 3\) structure shown in Fig. 5c. The fit to the data is shown in the supplementary note, and it is reasonable. The estimated moment size is *m* = 1.62(2) *μ*_{B} and the fitting quality are *χ*^{2} = 2.15 and *R*_{wp} = 42.6. It should be noted that the model is represented by 2 different IRs, Γ_{2} and Γ_{4} in Table 3. Another model is modulated all-in all-out structure as shown in Fig. 5d. This structure belongs to a single IR Γ_{2} in Table 3. The fit to the data is shown by the solid black curve in Fig. 3b and it is reasonable. The magnitude of the estimated moment size is 2.49(3)*μ*_{B}, and the fitting quality are *χ*^{2} = 1.72 and *R*_{wp} = 38.0. The moment sizes of neighboring spins are expressed as *m* cos*ϕ*, *m* cos(*ϕ* + 2/3*π*), *m* cos(*ϕ* + 4/3*π*)… Here the phase *ϕ* is arbitrary, and it cannot be determined by powder neutron diffraction.

### Phase diagram

CsCrF_{4} is originally a model material of the triangular spin tube, but the observation of the magnetic order in the present study reveals that the physics of the Kagome-Triangular (KT) lattice formed by the inter-tube interaction is important. Our analysis concluded that the LT phase is the quasi-120° structure at the L point in the first Brillouin zone, and the IT phase is \(\sqrt 3 \times \sqrt 3\) structure or modulated 120° structure at the H point. The LT structure is, however, different from the ground states expected in the Heisenberg KT lattice.^{20} The expected cuboc structure and 120° structure with ** k** =

**0**do not break three-fold rotational symmetry of the crystal. In contrast, the realized magnetic structure with \({\boldsymbol{k}} = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\), which corresponds to \({\boldsymbol{k}}_{{\mathrm{2}}D} = \left( {\frac{1}{2},0} \right)\), breaks the symmetry. Perturbation terms that induce the anisotropy, including DM interaction and/or single-ion anisotropy, are necessary. It is also noted that these terms stabilize a coplanar structure rather than a non-coplanar one. The magnitude of the DM vectors for both tube’s leg and rung are expected to be as small as 1–2% of the exchange interaction.

^{36}Nevertheless, the main kagome bond

*J*

_{2}, which has the exchange path of Cr

^{3+}−F

^{−}−F

^{−}−Cr

^{3+}, is also small, and the perturbation terms can be comparable to

*J*

_{2}. The perturbation terms as well as

*J*

_{2}are, thus, important for the selection of the ground state.

We classically calculated phase diagrams of the ground state of CsCrF_{4} using Luttinger-Tisza method.^{38,39} The Hamiltonian is as follows;

Here *l*_{α} is the position vector at *α*-site (*α* = A, B, and C) in the lattice ** l**, and

**is the unit vector of the crystal lattice along the**

*c**c*direction.

*z*

^{α}is the local

*z*-axis defined at the

*α*-site as shown in Fig. 1e. The sum is taken for

*l*_{α},

*l*_{β}, and \({\boldsymbol{l}}_\beta ^\prime\) all over the crystal, where

*α*≠

*β*and

**≠**

*l***′. The schematic exchange pathways are shown in Figs. 1d, e.**

*l**J*

_{0}and

*J*

_{1}are the exchange interactions of the tube’s leg and rung, respectively.

*J*

_{2}is the inter-tube interaction. The DM vector in the middle of the rung is

*d*_{1}, and it is along the

*c*axis.

^{36}The directions of the

*d*_{1}s are not determined but they are all up or all down. The DM vector in the middle of the leg

*d*_{0}is also allowed in the crystallographic symmetry.

*d*_{0}, however, induces an incommensurate spin correlation along the

*c*direction, which is not the case in CsCrF

_{4}. We, hence, ignore

*d*_{0}in our calculation. Another additional term, single-ion anisotropy

*D*, is also considered. The easy axes are assumed as the locally defined

*z*

^{α}-axes (

*α*= A, B, C) as shown in Fig. 1d so that the anisotropy terms preserve three-fold rotational symmetry in the

*ab*plane. The fixed values of

*J*

_{0}and

*J*

_{1}are used;

*J*

_{1}= 0.5 and

*J*

_{0}= 1.

^{40}In the calculation the

*J*

_{2},

*d*

_{1}and

*D*are much smaller than

*J*

_{0}and

*J*

_{1}, since Cr

^{3+}ion is isotropic and the bond length of

*J*

_{2}is long. The Hamiltonian in Eq. (3) is transformed into the wave vector space, and the eigenstates and eigenenergies are obtained by the diagonalization. The propagation vector of the ground state is obtained as the wave vector

**that gives the minimum eigenenergy. The magnetic structure is obtained from the corresponding eigenstate.**

*k*^{38,39}A constraint that the magnitude of the spins are the same was imposed.

Figure 6a shows the *d*_{1}−*J*_{2} phase diagram in the absence of the single-ion anisotropy *D*. When *J*_{2} is AF, i.e., *J*_{2} > 0, the ground state is 120° structure with \({\boldsymbol{k}} = \left( {0,0,\frac{1}{2}} \right)\), which we call the A′ structure (red symbols). The propagation vector corresponds to *k*_{2D} = (0, 0) in the *ab* plane. On the other hand, when *J*_{2} is FM the cuboc structure (green squares) exists even at very small *J*_{2} for |*d*_{1}| = 0. The DM interaction stabilizes a coplanar structure in the *ab* plane and destabilizes the cuboc structure. Indeed, at large |*d*_{1}| coplanar \(\sqrt 3 \times \sqrt 3\) structures with \({\boldsymbol{k}} = \left( {\frac{1}{3},\frac{1}{3},\frac{1}{2}} \right)\) or \({\boldsymbol{k}}_{{\mathrm{2}}D} = \left( {\frac{1}{3},\frac{1}{3}} \right)\), which we call the H structures (blue symbols), appears. Positive *d*_{1} induces negative chirality and negative *d*_{1} induces positive chirality for both A′ and H structures. In this phase diagram, the single-*k* 120° structure with \({\boldsymbol{k}} = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\) which is realized in CsCrF_{4}, does not exist.

Introduction of the single-ion anisotropy suppresses the non-coplanar cuboc structure and induces the single-*k* quasi-120° structure (orange symbols) in the range of *J*_{2} < 0, which we call the L structure, as shown in the *D*−*J*_{2} phase diagrams for *d*_{1} = 0 and −0.01 (Figs. 6b, c). The propagation vector is \({\kern 1pt} {\boldsymbol{k}} = \left( {\frac{1}{2},0,\frac{1}{2}} \right)\) or \({\boldsymbol{k}}_{{\mathrm{2}}D} = \left( {\frac{1}{2},0} \right)\), and the magnetic unit cell in the *ab* plane is doubled along the *a* direction. Because of the geometry of the easy axis, all-in all-out structure with the positive chirality, which is one of the candidates of the magnetic structure in the LT phase in Fig. 5a, is realized. In Fig. 6c the H structure with positive chirality, which coincides with a candidate in the IT phase in Fig. 5c, exists at small *D*. For *d*_{1} = 0.01, the DM interaction favoring negative chirality and the single-ion anisotropy favoring positive chirality compete to each other. The H structure with negative chirality exists in wide region, and the strong single-ion anisotropy induces the L structure indicated by the model A_{5} in Table 2. This magnetic structure is different from another candidate having negative chirality in the LT phase proposed by the experiment shown in Fig. 5b. For both cases where *d*_{1} = ±0.01, 120° structure with *k*_{2D} = (0, 0) is stable.

The triangle in the L structures in Figs. 6b–d is distorted due to *J*_{2}. It is, however, small; the most distorted case in the range of our calculation is that the angles between the neighboring spins are *ζ* = *η* = 117° and *ξ* = 127° at *J*_{2} = −0.03, *D* = −0.02, and *d*_{1} = −0.01.

## Discussion

One of the candidates for the magnetic structure of CsCrF_{4} in the LT phase is the L structure with positive chirality as shown in Fig. 5a. The appearance of the structure requires ferromagnetic Kagome bond *J*_{2} and single-ion anisotropy, and the DM interaction enhances the region of the structure in the *D* − *J*_{2} phase diagrams as shown in Figs. 6b, c. Another candidate, the L structure having negative chirality, is shown in Fig. 5b. The structure is, however, does not exist in our phase diagram. We, therefore, reject the candidate, and conclude that the all-in all-out structure in Fig. 5a is realized in the LT phase. The conclusion means that CsCrF_{4} is a rare experimental realization of the distortion free KT lattice having ferromagnetic Kagome bond.

Here we discuss the origin of the successive transition and the IT phase. The phase of the H structure and that of the L structure phase are adjacent in Fig. 6c. Suppose that CsCrF_{4} is in the H structure and in the vicinity of the phase boundary. Since the H structure covers the region of |*D*| < |*d*_{1}| in the phase diagram of the ground state, at finite temperatures of |*D*| < *k*_{B}*T* < |*d*_{1}|, the L structure is suppressed due to the thermal fluctuation, and the H structure is enhanced. This is a possible explanation for the appearance of the IT phase and the successive transition in CsCrF_{4}.

The \(\sqrt 3 \times \sqrt 3\) structure in the H structure is, however, represented by two different IRs, Γ_{2} and Γ_{4}, and its realization contradicts conventional Landau theory for second order phase transition. In this sense, the modulated all-in all-out structure in Fig. 5d is represented by the single IR Γ_{2} in Table 3, and its realization is more reasonable. This modulated structure is regarded that the spins component of the easy-axis direction in the \(\sqrt 3 \times \sqrt 3\) structure in Fig. 5c is statically ordered. The partially ordered 120° structure is, thus, more reasonable for the IT phase in the successive transition.

We discuss the reason why lambda-type anomaly was not observed in the heat capacity,^{34} even though the magnetic ordered state is realized. As shown in Fig. 2b, the strong magnetic diffuse scattering was observed at 10 K. This suggests that the short-range correlation of the spins is developed, and considerable amount of the magnetic entropy is consumed already at *T* > *T*_{N2}. At *T* ≤ *T*_{N2} in the IT phase, the magnetic diffuse scattering still remains. The result means that the entropy change at *T*_{N2} is small. At *T*_{N1} ≤ *T* ≤ *T*_{N2} the spin correlation is not long-ranged, and the correlation length gradually changes with the decrease of the temperature. The change of the entropy is, thus, smeared in wide temperature range in CsCrF_{4}, and the sharp anomaly was not detected in the heat capacity measurement.

Finally it should be noted that the threshold for the long-range order is determined by the experimental resolution, and, therefore, the possibility of short-range order with the correlation length longer than 800 Å cannot be excluded for the LT phase at *T* ≤ *T*_{N1}. In addition the dynamical spin correlation is not measured in the present neutron diffraction experiment. Possible short-range correlations in space and time in the LT phase also smears the change of the entropy.

In summary, we identified the magnetic states at low temperatures in a model material of triangular spin tubes coupled by the inter-tube interaction having KT geometry CsCrF_{4}. Magnetically ordered state was observed in contrast with previous studies. The quasi-120° structure with *k*_{2D} = (1/2, 0), which has not been predicted in theory in the category of the kagome lattice magnets, was experimentally identified. Single-ion anisotropy and DM interaction play important role for the selection of the magnetic structure. A successive phase transition was observed, and the magnetic structure in the IT phase is partially ordered 120° structure represented by *k*_{2D} = (1/3, 1/3). The IT phase is reasonably explained under the assumption that CsCrF_{4} is in the vicinity of the phase boundary in the *D* − *J*_{2} phase diagram. Since the key parameters, *J*_{2}, *D*, and *d*_{1}, are small in CsCrF_{4}, they can be controlled by, for example, pressure in extensive scales. In the system where a perturbation term has a casting vote for the selection of the state, external parameters including temperature, pressure, and magnetic field can induce various types of magnetic states. Further study in the wide range in the phase space will open a new window for the search of novel state of matter.

## Methods

High quality polycrystalline sample with the mass of 10 g was prepared by the solid state reaction method.^{34,35} The quality of the sample is discussed in the Supplementary Note 1. Lambda-type anomaly was not observed in the heat capacity measurement on the sample with the same quality as that used for neutron scattering experiment. Neutron diffraction experiments were carried out by the use of the powder neutron spectrometer ECHIDNA installed in the research reactor OPAL at ANSTO. Ge(331) monochromator was used and the neutron wavelength was *λ* = 2.4395 Å. The coverage of the scattering angle was 6° ≤ 2*θ* ≤ 165°. The measurement temperatures were *T* = 1.6 K, 1.75 K–3.5 K at intervals of 0.25 K, 4 K, 10 K and 100 K. A conventional liquid He cryostat was used to achieve the low temperatures. The Rietveld analysis was performed using the FULLPROF software package.^{41} To consider the candidates for the magnetic structure on the basis of the crystallographic space group and the magnetic propagation vector, the group theory method was used. Irreducible representations (IRs) were calculated using BasIreps in FullProf Suite.

## Data availability

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

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## Acknowledgements

We would like to thank T. Okubo, K. Seki and K. Okunishi for theoretical comment and discussions. Travel expenses to ANSTO for the neutron experiments were supported by General User Program for Neutron Scattering Experiments, Institute for Solid State Physics, The University of Tokyo (proposal no. 13559). This work was partly supported by a Grant-in-Aid for Scientific Research (No. 24340077) from the Ministry of Education, Culture, Sports, Science and Technology of Japan.

## Author information

### Affiliations

### Contributions

T.M. initiated and supervised the project. M.H. and T.M. wrote the manuscript. S.H. and H.K. joined in the discussion. M.A. performed neutron diffraction experiment. H.M. synthesize the sample. All the co-authors discussed the results and improved manuscript.

### Corresponding author

Correspondence to Takatsugu Masuda.

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