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 twodimensional network of the intertube interaction forms characteristic lattices. Among them KagomeTriangular (KT) lattice is known to exhibit an enriched phase diagram including various types of nontrivial structures: noncoplanar cuboc structure, coplanar 120° structure with the twodimensional 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 quasi120° 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 singleion anisotropy and DzyaloshinskiiMoriya 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 nontrivial magnetic state at low temperatures. Particularly the twodimensional (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 onedimensional (1D) systems quantum fluctuation as well as geometrical frustration induces nontrivial 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 nonmagnetic state having a unit of a twosite 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 TomonagaLuttinger 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 intertube interactions plays important roles. Particularly in the absences of frustration along the leg direction, the 2Dspin 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 intertriangular 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 KagomeTriangular (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 nextnearest 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 noncoplanar 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 FJ_{2} and AFJ_{1} is a multi Q structure having a 12sublattice with the spins directing along the 12middle 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 CrJarosites,^{23,24,25,26,27,28} the semimetals Mn_{3}Sn, Mn_{3}Ge,^{29} and rareearth 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 VJarosite.^{32} A material having FJ_{2} and AFJ_{1} which would exhibit nontrivial 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+} (3d^{3}) ions, which are JahnTeller inactive and carry Heisenberg spins, form an equilateral triangular tube along the crystallographic c direction. The space group is P6̄2m with a hexagonal structure, and the lattice is free from distortion down to low temperatures. In the CrF_{6} octahedron, the quasisquare 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 CrFCr 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 intertube 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 nondistorted KT lattice in Fig. 1b.^{22}
The magnetic susceptibility of CsCrF_{4} showed a broad maximum at T ~ 60 K, suggesting development of a shortrange antiferromagnetic spin correlation.^{34,35} Heat capacity showed no lambdatype 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 nonlinear 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 twodimensional geometry may have an important role.
In this paper, we demonstrate that nontrivial magnetic longrange 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 singleion anisotropy and DM interaction select a very rare magnetic structure, i.e., quasi120° 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 2θ ~ 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 shortrange correlation. At 100 K, in contrast, the broad peaks is suppressed, and paramagnetic diffuse scattering exists in the small 2θ.
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. Welldefined 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}. Twodimensional geometry of the intertube interaction is more important than the quantum nature of onedimensional spin tube. We, hence, found that CsCrF_{4} is an ideal model for the nondistorted 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 2θs 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 2θ 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 2θ = 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 longranged. 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 triplek 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 2θ = 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 P6̄2m 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 threefold 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 highsymmetry 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 LeviCivita 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 quasi120° 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 allin allout 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 cosϕ, m cos(ϕ + 2/3π), m cos(ϕ + 4/3π)… 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 KagomeTriangular (KT) lattice formed by the intertube interaction is important. Our analysis concluded that the LT phase is the quasi120° 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 threefold 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 singleion anisotropy, are necessary. It is also noted that these terms stabilize a coplanar structure rather than a noncoplanar 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 LuttingerTisza method.^{38,39} The Hamiltonian is as follows;
Here l_{α} is the position vector at αsite (α = A, B, and C) in the lattice l, and c is the unit vector of the crystal lattice along the c direction. z^{α} is the local zaxis defined at the αsite 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 ≠ l′. The schematic exchange pathways are shown in Figs. 1d, e. J_{0} and J_{1} are the exchange interactions of the tube’s leg and rung, respectively. J_{2} is the intertube 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, singleion 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 threefold 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 k that gives the minimum eigenenergy. The magnetic structure is obtained from the corresponding eigenstate.^{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 singleion 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 singlek 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 singleion anisotropy suppresses the noncoplanar cuboc structure and induces the singlek quasi120° 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, allin allout 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 singleion anisotropy favoring positive chirality compete to each other. The H structure with negative chirality exists in wide region, and the strong singleion 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 singleion 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 allin allout 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 allin allout 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 easyaxis 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 lambdatype 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 shortrange 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 longranged, 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 longrange order is determined by the experimental resolution, and, therefore, the possibility of shortrange 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 shortrange 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 intertube interaction having KT geometry CsCrF_{4}. Magnetically ordered state was observed in contrast with previous studies. The quasi120° 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. Singleion 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. Lambdatype 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° ≤ 2θ ≤ 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 GrantinAid for Scientific Research (No. 24340077) from the Ministry of Education, Culture, Sports, Science and Technology of Japan.
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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 coauthors discussed the results and improved manuscript.
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Hagihala, M., Hayashida, S., Avdeev, M. et al. Magnetic states of coupled spin tubes with frustrated geometry in CsCrF_{4}. npj Quantum Mater. 4, 14 (2019). https://doi.org/10.1038/s4153501901525
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