A series of magnon crystals appearing under ultrahigh magnetic fields in a kagomé antiferromagnet


Geometrical frustration and a high magnetic field are two key factors for realizing unconventional quantum states in magnetic materials. Specifically, conventional magnetic order can potentially be destroyed by competing interactions and may be replaced by an exotic state that is characterized in terms of quasiparticles called magnons, the density and chemical potential of which are controlled by the magnetic field. Here we show that a synthetic copper mineral, Cd-kapellasite, which comprises a kagomé lattice consisting of corner-sharing triangles of spin-1/2 Cu2+ ions, exhibits an unprecedented series of fractional magnetization plateaus in ultrahigh magnetic fields of up to 160 T. We propose that these quantum states can be interpreted as crystallizations of emergent magnons localized on the hexagon of the kagomé lattice.


Quantum many-body systems accommodate various exotic states and phenomena. One of the most notable examples is Bose–Einstein condensation (BEC), where a macroscopic number of bosonic particles occupy a single particle state as in a superfluid state of liquid 4He and in cold atomic gases. With the aid of attractive force, fermions in pairs can also condensate as in a superconducting state of electrons. In most antiferromagnetic insulators, the elementary excitation is a bosonic excitation magnon, and this can form a BEC1,2,3. Interestingly, interactions between magnons and couplings with the basal crystalline lattice lead to rich physics in quantum antiferromagnets, thereby distinguishing it from the canonical BEC.

The magnon picture has proven extremely fruitful for several antiferromagnets composed of spin-1/2 pairs with a spin-singlet (S = 0) ground-state, and triplet (S = 1) excitations called triplons. The triplons are similar to conventional magnons excited in an ordered antiferromagnet because both carry the spin angular momentum of ħ, and thus the two terms are occasionally used interchangeably2,3. At a critical applied magnetic field, the energy of one of the Zeeman-split triplet components intersects the ground-state singlet, thereby resulting in a long-range magnetic order. Specifically, the transition corresponds to a BEC of diluted triplons (magnons), and this is typically observed in TlCuCl34,5. Above the critical field, the magnetization starts to increase linearly when the density of magnons increases with magnetic field. The magnetic field acts as a chemical potential for magnons, and thus controls the density of the magnons (which is proportional to the magnetization).

In simple spin systems, the magnetization increases smoothly with the magnetic field and eventually saturates. However, in certain quantum magnets, flat regions termed as magnetization plateaus appear at fractional magnetizations before saturation. There are two types of magnetization plateaus: a classical one that is described by a collinear arrangement of classical spins and a quantum state comprising entangled spins6. Classical magnetization plateaus are observed in triangular magnets, such as Cs2CuBr47 and Ba3CoSb2O98,9, and the quantum plateaus in dimer magnets such as NH4CuCl310 and SrCu2(BO3)211.

A transition to a quantum plateau as a function of magnetic field is considered to be a superfluid-insulator transition of hard-core bosons (magnons). Interacting magnons in a BEC state tend to localize due to the suppression of kinetic energy and eventually crystallize to become “insulating” such as Mott insulators in strongly correlated electron systems12. The magnon crystal exhibits a fixed density of magnons, and thus the magnetization remains at a fractional value of the full magnetization in a field range6. The fractional value of magnetization is attributed to the commensurability of the magnon crystal when there is no topological order. The number of magnons, QmagS(1 – m), in the magnetic unit cell should be an integer where Qmag, S, m denote the number of spins in the magnetic unit cell, the spin quantum number, and the magnetization divided by the saturation magnetization, respectively13. In SrCu2(BO3)2, which comprises pairs of Cu2+ ions arranged orthogonally to each other in the sheet to form a Shastry–Sutherland lattice11, a series of magnetization plateaus appear at m = 1/8, 1/4, 1/3 (Qmag = 16, 8, 12)14,15; and nuclear magnetic resonance measurements directly confirmed spontaneous translational symmetry breaking in the magnon crystals16.

In the spin-1/2 kagomé antiferromagnet (KAFM)17,19,19, the ground-state is a gapless or gapful spin liquid and the formation of nontrivial magnons is theoretically expected immediately below the saturation20. When the magnetic field is set to infinitesimally smaller than the saturation field Bs, a magnon with total Sz = 2 in a hexagonal plaquette is generated in the fully polarized spin state, which is the vacuum of magnons as schematically depicted in Fig. 1. Each spin inside the hexagonal plaquette equally carries fractional magnetization, and thus, the ‘hexagonal magnon’’ corresponds to a highly quantum mechanical entity. Given the absence of energy cost for magnon generation, the density rapidly increases to 1/9 before the magnons overlap with each other to feel mutual repulsion. This results in an decrease in the magnetization from 1 to 7/9 at Bs20. Subsequently, a crystalline phase with a superstructure of the \(\sqrt 3\) × \(\sqrt 3\) unit cell with Qmag = 9 is formed in a range of fields, thereby yielding a 7/9 magnetization plateau. A large magnon is emergently generated on a hexagon of the kagomé lattice in the KAFM, which is significantly different from dimer magnets with singlet and triplet states that naturally occur on built-in pairs of Cu ions.

Fig. 1

Calculated magnetization process for the spin-1/2 KAFM with the nearest-neighbor interaction J. The tensor network method with the projected entangled pair state (PEPS) is used. The vertical and horizontal axes represent magnetization M divided by saturated magnetization Ms and magnetic field B divided by J, respectively. The top left inset shows a schematic drawing of hexagonal magnons that are depicted by doughnuts containing six entangled spins. The other intervening spins point upward in the direction of magnetic field. The magnon crystal forms a superlattice with a √3 × √3 unit cell. The bottom right inset shows hexagonal magnons expected to appear at the 1/3, 5/9, and 7/9 plateaus. In the upper part, the magnons are defined by the total spin Sz = 0, 1, and 2 for the six spins on the hexagon, respectively, while in the lower part based on the magnon picture, the number of magnons correspond to 3 (hexagon + double circle), 2 (single circle), and 1 (only hexagon), respectively. Using the bracket notation, the one-magnon state with Sz = 2 is expressed as \({\sum }_{i = 1}^6 \left( { - 1} \right)^iS_i^ - |0 > \), where the sum is obtained inside the hexagon, and \(|0 > \) denotes the saturated state

Here, we report the observation of a series of fractional magnetization plateaus in the kagomé antiferromagnet Cd-kapellasite (CdK) and demonstrate the presence of emergent hexagonal magnons in the kagomé lattice. Some of the observed magnetization plateaus are reproduced by theoretical calculations for the simple KAFM model, while the others may be stabilized by lattice commensurability, additional long-range interactions, and potentially coupling to lattice.


Theoretical predictions for multiple plateaus

Recent calculations by the density-matrix-renormalization-group method, the exact diagonalization, and the tensor network method show that in addition to the well-established 7/9 plateau, three plateaus appear at m = 5/9, 1/3, 1/921,23,24,24. It is also suggested21,23,23 that the 5/9 and 1/3 plateaus are magnon crystals with Qmag = 9, which are similar to that at m = 7/9 but with Sz = 1 and 0, respectively, as depicted in Fig. 1; the 1/9 plateau is supposed to be another state, possibly a spin liquid with topological order21. However, one must be careful in concluding this because there are many competing phases in highly frustrated systems. In the present study, we calculated the complete magnetization process in the extended projected entangled pair states (PEPS) scheme, and found three plateaus at m = 1/3, 5/9, 7/9, as shown in Fig. 1, which supports the previous results as shown in Fig. 1. Additionally, we examined the magnetic structure at the 1/3 plateau and observed that a magnon crystal composed of hexagonal magnons with Sz = 0 in the \(\sqrt 3\) × \(\sqrt 3\) structure was associated with the lowest energy among other competing states such as the up-up-down state (Supplementary Fig. 1). Thus, the hexagonal magnon must correspond to an entity that should be realized under the magnetic field for the KAFM, and this should be experimentally evidenced.

Experimental obstacles

Despite the intriguing predictions for the KAFM in magnetic fields, there is a paucity of experimental evidence due to the lack of ideal model compounds, and also the difficulties in experiments under high fields. Real materials always suffer from lattice distortion25 or disorder26, and this tends to mask the intrinsic magnetism of the KAFM. The best-characterized S = 1/2 KAFM is herbertsmithite with a large interaction of J ~ 200 K27, and this implies that ultrahigh magnetic fields not <Bs = 400 T are necessary to record the complete magnetization process. However, experimentally available static magnetic fields are only below 45 T and typical pulsed magnetic fields are limited to below 100 T28. Furthermore, magnetization measurements by the conventional induction method are only available in pulsed magnetic fields below 100 T in the short time duration corresponding to several milliseconds;28 for a larger pulsed field, a much shorter time window of several microseconds is available, which causes a large electromagnetic noise preventing facile magnetization measurements. On the other hand, a state-of-the-art measurement using a Faraday rotation technique made it possible to record the complete magnetization process of CdCr2O4 up to 140 T, and this revealed a spin-nematic phase just below the saturation field29. In order to unveil the physics of the KAFM, both a suitable model compound with a relatively low-saturation field around 100 T and an improvement in the Faraday rotation technique are necessary. It is noted that the required low-temperature condition, T « J/kB, is difficult to achieve for a compound with small J and Bs values.

Kagomé antiferromagnet CdK

To study the magnetism of S = 1/2 KAFM under magnetic fields, we selected Cd-kapellasite (CdK), CdCu3(OH)6(NO3)2·H2O30, which is isostructural to kapellasite, ZnCu3(OH)6Cl231. The compound has a quasi-two-dimensional structure with an undistorted kagomé lattice of Cu2+ ions and a moderate antiferromagnetic interaction of J ~ 45 K (Bs ~ 100 T) (Fig. 2a)32. The ground-state of CdK is not a spin liquid but a long-range order (LRO) with a q = 0 structure (a negative vector chirality order) below TN ~ 4 K, which must be induced by a Dzyaloshinskii–Moriya (DM) interaction with a magnitude of approximately 10% of J. Other possible perturbations are the next-nearest-neighbor interaction J2 and diagonal interaction Jd bridged via the Cd ion in the center of the hexagon as shown in Fig. 2b, which was observed as a low value (Supplementary Fig. 2).

Fig. 2

Crystal structure and magnetic interactions of CdK. a Kagomé layers comprising Cu2+ and Cd2+ ions possess good two dimensionality and are separated by nonmagnetic nitrate ions and crystalline water molecules. b Regular kagomé lattice composed of spin-1/2 Cu2+ ions with a Cd ion in the center of each hexagon. Magnetic interactions between spins are nearest-neighbor J, a Dzyaloshinskii–Moriya (DM) interaction as large as 10% of J, small next-nearest-neighbor interaction J2, and diagonal interaction Jd across the Cd ion in the hexagon

Faraday rotation measurements up to 160 T

We measured small magnetization from a tiny hexagonal single crystal of CdK with a diameter of approximately 1 mm and a thickness of 150 µm (Fig. 3a) by a Faraday rotation technique optimized to a single-turn coil in magnetic fields of up to 160 T. The experimental set-up and results are shown in Fig. 3b. The polarization angle of an incident light with λ = 532 nm (Supplementary Fig. 3) was rotated with a varying magnetic field in several microseconds via the Faraday effect from induced magnetization in the sample (Fig. 3c). Figure 3d shows magnetizations converted from the data in descending pulsed magnetic fields (Supplementary Fig. 4). The magnetization curve measured at 8 K smoothly increased and saturated at approximately 150 T. At 6 K, a faint wiggling was observed, which seemed to produce many anomalies at 5 K.

Fig. 3

Magnetization measurements by the Faraday rotation technique in pulsed magnetic fields up to 160 T. a Single crystal of CdK on a sapphire disk substrate used in high-field Faraday rotation measurements. The crystal exhibits a flat (001) surface that effectively reduces scattering of light and is sufficiently large to obtain a Faraday rotation signal. b Schematic illustration of the experimental set-up. A high-magnetic field is generated inside a single-turn coil of 12 mm inner diameter by injecting a huge electric current (2–3 mega-ampere). c Typical time evolutions of a pulsed magnetic field with a maximum at 160 T and a time duration of 7 µs and Ip and Is at 5 K. The hexagonal plate-like single crystal of CdK shown in a mounted on a sapphire substrate is placed in the coil such that the magnetic field is perpendicular to the hexagonal surface (B /// c). Linearly polarized incident light comes from the left and passes through the crystal. A change in the polarization angle due to the Faraday effect in the magnetized crystal is measured: transmitted light is split into vertical and horizontal components, Ip and Is, and each intensity is recorded by an oscilloscope. d Field dependences of the Faraday rotation angle θF and the corresponding magnetizations at 5 K (purple), 6 K (yellow), and 8 K (blue-green). For clarity, offsets of 20 and 50 degrees are added to the data at 6 and 8 K, respectively. The magnetization data from the Faraday rotation angle are calibrated to reproduce those obtained by the induction method by using a nondestructive pulse magnet as denoted by the black line below 55 T at 4.2 K. The large noises at approximately 30 T in the data at 6 and 8 K and at approximately 50 T in the data at 5 K are due to reductions in intensity for either Ip or Is at the rotation angle corresponding to 90 degree

Figure 4a shows the magnetization process at 5 K and its field derivative, which is compared with the calculated magnetization process in the presence of DM interaction. Below 0.4 µB, the experimental magnetization is in good agreement with the calculation and deviates above that. At least seven anomalies are observed at magnetizations exceeding 0.4 µB. Above Bs = 160 T, M reaches 1.15 µB/Cu, and this was nearly equal to the saturation magnetization with fully polarized spins: gSµB with gc ~ 2.3 from magnetic susceptibility (Supplementary Fig. 2).

Fig. 4

Appearance of multiple magnetization plateaus in CdK. a Field dependences of magnetization and its derivative at 5 K and B // c. The purple and yellow-green lines represent magnetizations measured by the Faraday rotation and induction method, respectively, and blue-green and black points denote the field derivative of the former and latter curve, respectively. The magnitudes of B and M at seven local minima in the field derivative curve are termed as Bk and Mk as shown by the broken lines, which can correspond to a series of magnetization plateaus. The saturation field Bs = 160 T is determined at which M reaches the full magnetization Ms = 1.15 µB. The green line shows the M calculated by PEPS for an S = 1/2 KAFM model with J = 45 K and the z component of DM interaction of 0.1 J. b Comparison between experimentally observed plateau magnetizations mk = Mk/Ms and fractional magnetizations expected from the series of magnon crystals with Qmag = 9, 12, 21, 36 unit cells as shown in Fig. 5. The fractions in the red bold letter are close to one of the mk values while the fractions in regular blue font cannot be observed with the exception of 30/36 that is assigned to 10/12

Magnetization plateaus

We consider the anomalies as a series of blunt plateaus that were blurred or inclined due to the finite temperature effect or anisotropy such as DM interaction. In conventional ordered antiferromagnets a metamagnetic transition or a spin-flop transition can occur in a magnetic field. However, weak anisotropy in Cu2+ spin systems makes it difficult for such transitions to occur. We consider blunting by temperature and define a critical field Bk and a magnetization Mk for each plateau at which the differential magnetization takes a local minimum; the Bk should correspond to the center of the field range for the plateau. The obtained values of [Bk (T), Mk (µB/Cu), mk] (mk = Mk/1.15) are (47.6, 0.42, 0.37), (72.6, 0.59, 0.51), (95.3, 0.78, 0.68), (113.8, 0.94, 0.81), (121.6, 0.98, 0.85), (129.1, 1.04, 0.9), and (139.7, 1.08, 0.94) for k = 1–7, respectively. It should be noted that the anomalies are distinct for k = 2, 3, 4, and 7 and weaker for k = 5 and 6. As mentioned above, it is expected that magnetization plateaus from magnon crystals with Qmag = 9 appear only at m = 1/3, 5/9, and 7/9 for the simple KAFM. The values were near to m1, m2, and m4, as shown in Fig. 4b, although they significantly deviated from them. The present observation of the increased number of plateaus in CdK significantly indicate the formation of other types of magnon crystals with unit cells exceeding Qmag = 9.


We considered possible magnetic structures realized at the magnetization plateaus in CdK. As in the case of the simple KAFM, we assumed that a type of localized hexagonal magnons is periodically aligned to reduce mutual repulsion while maintaining a sixfold rotational symmetry. Subsequently, such a series of magnon crystals as shown in Fig. 5 with unit cells of Qmag = 9, 12, 21, 36 can appear wherein each involves three sequences with 1–3 magnons on the hexagon. All the experimentally observed mk values are well reproduced. For example, m7 = 0.94 near the saturation is close to 34/36 ~ 0.944, and m6 = 0.90 is nearly equal to 19/21 ~ 0.905. Furthermore, m5 = 0.85, m4 = 0.82, m3 = 0.68, m2 = 0.51, and m1 = 0.37 are near 5/6 ~ 0.833, 17/21 ~ 0.810, 2/3 ~ 0.667, 1/2 = 0.5, and 1/3 ~ 0.333, respectively (Fig. 4b). Thus, one from the Qmag = 9 series, three from Qmag = 12, two from Qmag = 21, and one from Qmag = 36 were observed. The fact that all the three sequences appeared for Qmag = 12 while only part appeared for the others prompted us to determine a rule for the magnon crystallization in CdK.

Fig. 5

Possible series of magnetic structures for the magnon crystals with Qmag = 9, 12, 21, and 36. Among them, those corresponding to the observed seven magnetization plateaus are emphasized. Red hexagons denote localized hexagonal magnons with the total Sz = 0, 1, and 2. Other intervening spins are fully polarized along the magnetic field as shown for Qmag = 9 in the inset of Fig. 1. Blue dotted lozenges represent magnetic unit cells

Emergence of larger unit cells in CdK must be attributed to additional farther–neighbor interactions such as J2 and Jd. Our calculations of magnetization without them and with 10% DM interaction does not exhibit any anomalies after an inclined 1/3 plateau with increasing fields (Fig. 4a). It is emphasized that the anomalies in CdK appear when the experimental magnetization curve deviates from the theoretical one, which suggests that effects excluded in the calculation play a crucial role. If J2 works as an effective repulsion among magnons, the Qmag = 9 structure must become unstable (Supplementary Fig. 5). For the Qmag = 12 structure, on the other hand, J2 does not work while Jd does. The experimental fact that all the three sequences are observed for the Qmag = 12 series and only a part for the others (e.g., not 5/9 but 6/12 for m2) indicates the relative stability of Qmag = 12. This implies repulsive (ferromagnetic) J2 and attractive (antiferromagnetic) Jd. Larger unit cells, such as Qmag = 21 and 36, can be stabilized by weak farther–neighbor interactions or the enlargement of the effective size of hexagonal magnons. Therefore, the appearance of multiple magnetization plateaus in CdK is reasonably explained by assuming a series of magnon crystals in a spin-1/2 KAFM with additional interactions.

Finally, we focus on the reason for the appearance of magnetization plateaus in CdK after the deviation from the calculation based on the J + DM model; the smooth rise of the calculated curve indicates that spins are gradually forced to align along the magnetic field from the coplanar q = 0 structure as expected for a classical spin system. One possibility is the magnetostriction that induces a lattice distortion33. For example, a hexagon where a localized magnon lives can deform to increase antiferromagnetic J, and thereby to stabilize a local magnon. When this type of a lattice distortion occurs periodically to form a superstructure, hexagonal magnons tend to crystallize at high fields with m ≥ 1/3. Therefore, a spin-lattice coupling potentially makes a tilted q = 0 magnetic structure unfavorable and leads to a series of crystallizations of localized magnons with the aid of farther–neighbor interactions.


Sample preparation

Single crystals of Cd-kapellasite, CdCu3(OH)6(NO3)2·H2O, were synthesized by a two-step hydrothermal method32. A quartz ampoule with a length of 150 mm was filled with ingredients (Cu(OH)2: 0.1 g, Cd(NO3)2•4H2O: 5 g, H2O: 4 g) and sealed. A thick quartz tube with outer and inner diameters of 12 and 8 mm, respectively, was used to avoid bursting due to increased pressure inside the tube during heat treatment. The ampoule was placed horizontally in a two-zone furnace and heated to 180 °C at the hot end and to 130 °C at the cold end for a week. Polycrystalline samples of CdK were quickly produced over the tube and subsequently slowly transported into the cold zone to condense into a bunch of single crystals 100 µm in diameter. After all polycrystalline samples were transported to the cold zone, the temperature gradient was reversed. The ex-cool zone was set to 160 °C, and the ex-hot zone was set to 140 °C. This resulted in inverse transportation, thereby resulting in the growth of hexagonal plate-like crystals as large as 1 mm in diameter and 150 µm in thickness as typically shown in Fig. 3a.

Magnetization measurements

Magnetization measurements in low-magnetic fields below 7 T were conducted by using a single crystal of CdK with a weight of 2.38 mg in a Magnetic-Property-Measurement-System 3 (MPMS-3, Quantum Design). Magnetic susceptibilities along the a and c axes were measured at the constant field of 1 T. Magnetization at pulsed magnetic fields up to 60 T was measured at 4.2 K on stacked single crystals via the electromagnetic induction method. The absolute value of magnetization was calibrated by the data obtained from MPMS-3.

Faraday rotation measurements in pulsed magnetic fields

A single-turn coil as shown in Fig. 3a was used to generate ultrahigh magnetic fields up to 160 T34. A sample was not destroyed after the experiment because the coil explodes outwards along the direction of Maxwell stress. Faraday rotation was measured in a short time duration corresponding to 7 µs. The sample temperature was set to 5, 6, and 8 K and could slightly change at elevated fields due to the magnetocaloric effect in the adiabatic condition. A change in the polarization angle θF was proportional to magnetization M induced by the applied field in the sample: θF = αMd where α denotes the Verdet constant and d denotes the thickness of the sample. Specifically, θF is calculated from the intensities of the vertical and horizontal components, Ip and Is, by the formula: θF = cos−1 {(Ip − Is)/(Ip + Is)}.

Tensor network calculations

Magnetization process of a S = 1/2 KAFM with the nearest-neighbor interaction J is calculated by the infinite projected entangled pair state (iPEPS)35,37,37 method that expresses a wave function as an extended tensor product state termed as the projected simplex pair state (PESS)38,39. Unit cells up to 18 sites are assumed. The wave function is optimized by the simple update method40,41 with bond dimensions D = 4–7. Physical quantities were typically calculated by the corner transfer matrix method42 with bond dimensions χ = D2.

Data availability

The publication data used in this study is available on https://doi.org/10.6084/m9.figshare.7609745.v1. The data files are also available from the corresponding author upon request. The source data underlying Figs. 1, 3c, d, and 4a, and Supplementary Figures 14 are provided as a Source Data file.


  1. 1.

    Matsubara, T. & Matsuda, H. A lattice model of liquid helium, I. Prog. Theor. Phys. 16, 569–582 (1956).

  2. 2.

    Giamarchi, T., Rüegg, C. & Tchernyshyov, O. Bose–Einstein condensation in magnetic insulators. Nat. Phys. 4, 198–204 (2008).

  3. 3.

    Zapf, V., Jaime, M. & Batista, C. D. Bose-Einstein condensation in quantum magnets. Rev. Mod. Phys. 86, 563–614 (2014).

  4. 4.

    Nikuni, T. et al. Bose-Einstein condensation of dilute magnons in TlCuCl3. Phys. Rev. Lett. 84, 5868–5871 (2000).

  5. 5.

    Rüegg, Ch. et al. Bose–Einstein condensation of the triplet states in the magnetic insulator TlCuCl3. Nature 423, 62–65 (2003).

  6. 6.

    Takigawa, M. & Mila, F. in Introduction to Frustrated Magnetism (eds. Lacroix, C. et al.) 241–267 (Springer, Berlin Heidelberg, 2011).

  7. 7.

    Fortune, N. A. et al. Cascade of magnetic-field-induced quantum phase transitions in a spin-1/2 triangular-lattice antiferro-magnet. Phys. Rev. Lett. 102, 257201 (2009).

  8. 8.

    Zhou, H. D. et al. Successive phase transitions and extended spin-excitation continuum in the S=1/2 triangular-lattice antiferromagnet Ba3CoSb2O9. Phys. Rev. Lett. 109, 267206 (2012).

  9. 9.

    Shirata, Y. et al. Experimental realization of a spin-1/2 triangular-lattice Heisenberg antiferromagnet. Phys. Rev. Lett. 108, 057205 (2012).

  10. 10.

    Shiramura, W. et al. Magnetization plateaus in NH4CuCl3. J. Phys. Soc. Jpn 67, 1548–1551 (1998).

  11. 11.

    Kageyama, H. et al. Exact dimer ground state and quantized magnetization plateaus in the two-dimensional spin system SrCu2(BO3)2. Phys. Rev. Lett. 82, 3168–3171 (1999).

  12. 12.

    Imada, M., Atsushi, F. & Tokura, Y. Metal-insulator transitions. Rev. Mod. Phys. 70, 1039–1263 (1998).

  13. 13.

    Oshikawa, M., Yamanaka, M. & Affleck, I. Magnetization plateaus in spin chains: “Haldane gap” for half-integer spins. Phys. Rev. Lett. 78, 1984–1987 (1997).

  14. 14.

    Matsuda, Y. H. et al. Magnetization of SrCu2(BO3)2 in ultrahigh magnetic fields up to 118 T. Phys. Rev. Lett. 111, 137204 (2013).

  15. 15.

    Kodama, K. et al. Magnetic superstructure in the two-dimensional quantum antiferromagnet SrCu2(BO3)2. Science 298, 395–399 (2002).

  16. 16.

    Yan, S., Huse, D. A. & White, S. R. Spin-liquid ground state of the S = 1/2 kagome Heisenberg antiferromagnet. Science 332, 1173–1176 (2011).

  17. 17.

    He, Y. -C. et al. Signatures of Dirac cones in a DMRG study of the kagome Heisenberg model. Phys. Rev. X 7, 031020 (2017).

  18. 18.

    Liao, H. -J. et al. Gapless spin-liquid ground state in the S = 1/2 kagome antiferromagnet. Phys. Rev. Lett. 118, 137202 (2017).

  19. 19.

    Schulenburg, J. et al. Macroscopic magnetization jumps due to independent magnons in frustrated quantum spin lattices. Phys. Rev. Lett. 88, 167207 (2002).

  20. 20.

    Nishimoto, S., Shibata, N. & Hotta, C. Controlling frustrated liquids and solids with an applied field in a kagome Heisenberg antiferromagnet. Nat. Commun. 4, 2287 (2012).

  21. 21.

    Capponi, S. et al. Numerical study of magnetization plateaus in the spin-1/2 kagome Heisenberg antiferromagnet. Phys. Rev. B 88, 144416 (2013).

  22. 22.

    Chen, Xi et al. Thermodynamics of spin-1/2 Kagomé Heisenberg antiferromagnet: algebraic paramagnetic liquid and finite-temperature phase diagram. Sci. Bull. 63, 1545–1550 (2018).

  23. 23.

    Picot, T. et al. Spin-S kagome quantum antiferromagnets in a field with tensor networks. Phys. Rev. Lett. 93, 060407 (2016).

  24. 24.

    Hiroi, Z. et al. Spin-1/2 kagomé-like lattice in volborthite Cu3V2O7(OH)2· 2H2O. J. Phys. Soc. Jpn 70, 3377–3384 (2001).

  25. 25.

    Kawamura, H., Watanabe, K. & Shimokawa, T. Quantum spin-liquid behavior in the spin-1/2 random-bond Heisenberg antiferromagnet on the kagome lattice. J. Phys. Soc. Jpn 83, 103704 (2014).

  26. 26.

    Shores, M. P. et al. A structurally perfect S = 1/2 kagome antiferromagnet. J. Am. Chem. Soc. 127, 13462–13463 (2005).

  27. 27.

    N. Miura & F. Herlach. in Springer Topics in Applied Physics (ed. Herlach, F.) 247–350, Vol. 57 (Springer, Berlin, 1985).

  28. 28.

    Miyata, A., Takeyama, S. & Ueda, H. Magnetic superfluid state in the frustrated spinel oxide CdCr2O4 revealed by ultrahigh magnetic fields. Phys. Rev. B 87, 214424 (2013).

  29. 29.

    Nytko, E. A. et al. CdCu3(OH)6(NO3)2: An S = 1/2 Kagomé Antiferromagnet. Inorg. Chem. 48, 7782–7786 (2009).

  30. 30.

    Fåk, B. et al. Kapellasite: A kagome quantum spin liquid with competing interactions. Phys. Rev. Lett. 109, 037208 (2012).

  31. 31.

    Okuma, R. et al. Weak ferromagnetic order breaking the threefold rotational symmetry of the underlying kagome lattice in CdCu3(OH)6(NO3)2·H2O. Phys. Rev. B 95, 094427 (2017).

  32. 32.

    Becca, F. & Mila, F. Peierls-like transition induced by frustration in a two-dimensional antiferromagnet. Phys. Rev. Lett. 89, 037204 (2002).

  33. 33.

    Miura, N., Osada, T. & Takeyama, S. Research in super-high pulsed magnetic fields at the megagauss laboratory of the University of Tokyo. J. Low. Temp. Phys. 133, 139–158 (2003).

  34. 34.

    Verstraete, F. & Cirac, J. I. Valence-bond states for quantum computation. Phys. Rev. A 70, 060302 (2004).

  35. 35.

    Verstraete, F. & Cirac, J. I. Renormalization algorithms for quantum-many body systems in two and higher dimensions. Preprint at http://arXiv.org/abs/cond-mat/0407066 (2004).

  36. 36.

    Jordan, J., Orus, R., Vidal, G., Verstraete, F. & Cirac, J. I. Classical simulation of infinite-size quantum lattice systems in two spatial dimensions. Phys. Rev. Lett. 101, 250602 (2008).

  37. 37.

    Poilblanc, D. et al. Simplex Z2 spin liquids on the kagome lattice with projected entangled pair states: Spinon and vison coherence lengths, topological entropy, and gapless edge modes. Phys. Rev. B 87, 140407(R) (2012).

  38. 38.

    Xie, Z. Y. et al. Tensor renormalization of Quantum Many-Body Systems using projected entangled simplex states. Phys. Rev. X 4, 011025 (2014).

  39. 39.

    Jiang, H. C., Weng, Z. Y. & Xiang, T. Accurate determination of tensor network state of Quantum lattice models in two dimensions. Phys. Rev. Lett. 101, 090603 (2008).

  40. 40.

    Okubo, T. et al. Ground-state properties of Na2IrO3 determined from an ab initio Hamiltonian and its extensions containing Kitaev and extended Heisenberg interactions. Phys. Rev. B 96, 054434 (2017).

  41. 41.

    Oru ́s, R. & Vidal, G. Simulation of two-dimensional quantum systems on an infinite lattice revisited: Corner transfer matrix for tensor contraction. Phys. Rev. B 80, 094403 (2009).

  42. 42.

    Nishino, T. & Okunishi, K. Corner transfer matrix renormalization group method. J. Phys. Soc. Jpn 65, 891–894 (1996).

Download references


We are grateful to T. Misawa, H. Tsunetsugu, and C. Hotta for helpful discussion. R.O. is supported by the Materials Education Program for the Future Leaders in Research, Industry, and Technology (MERIT) under the Ministry of Education, Culture, Sports, Science, and Technology of Japan (MEXT). The study was partially supported by KAKENHI (Grant No. 15K17701), the Core-to-Core Program for Advanced Research Networks under the Japan Society for the Promotion of Science (JSPS), and MEXT of Japan as a social and scientific priority issue (Creation of new functional devices and high-performance materials to support next-generation industries; CDMSI) to be solved by using post-K computer and “Exploratory Challenge on Post-K computer” (Challenge of Basic Science–Exploring Extremes through Multi-Physics and Multi-Scale Simulations).

Author information

R.O., D.N., S.T., and Z.H. conceived and designed the study. A. Miyake and A. Matsuo measured the magnetization curve up to 60 T under supervision of M.T.; K.K., R.O., D.N. measured the magnetization curve up to 180 T under supervision of S.T.; R.O., D.N., S.T., and Z.H. interpreted the experimental data. T.O. performed and interpreted PEPS calculations under supervision of N.K.; R.O. wrote the manuscript. All authors discussed and commented on the manuscript.

Correspondence to R. Okuma.

Ethics declarations

Competing interests

The authors declare no competing interests.

Additional information

Journal peer review information: Nature Communications thanks Vivien Zapf and the other anonymous reviewer(s) for their contribution to the peer review of this work. Peer reviewer reports are available.

Publisher’s note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

Supplementary information

Rights and permissions

Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.

Reprints and Permissions

About this article

Verify currency and authenticity via CrossMark

Cite this article

Okuma, R., Nakamura, D., Okubo, T. et al. A series of magnon crystals appearing under ultrahigh magnetic fields in a kagomé antiferromagnet. Nat Commun 10, 1229 (2019). https://doi.org/10.1038/s41467-019-09063-7

Download citation

Further reading


By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.