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The Magnetic Susceptibility Bifurcation in the NiDoped Sb_{2}Te_{3} Topological Insulator with Antiferromagnetic Order Accompanied by Weak Ferromagnetic Alignment
Nanoscale Research Letters volume 16, Article number: 180 (2021)
Abstract
The magnetic susceptibility reveals a discontinuity at Néel temperature and a hysteresis loop with low coercive field was observed below Néel temperature. The magnetic susceptibility of zero field cool and field cool processes coincide at a temperature above the discontinuity, and they split at temperature blow the discontinuity. The magnetic susceptibility splitting is larger at lower external magnetic fields. No more magnetic susceptibility splitting was observed at a magnetic field above 7000 Oe which is consistent with the magnetic anisotropy energy. Our study supports that these magnetic susceptibility characteristics originate from an antiferromagnetic order accompanied by weak ferromagnetism.
Introduction
Threedimensional topological insulators possess a linear dispersion gapless surface state that is protected by timereversal symmetry [1, 2]. The topological surface state consists of spinfiltered Dirac fermions. This spin helical texture of the topological surface state has attracted a great deal of attention due to its possible electric and spinrelated applications [3,4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20]. Aside from the intrinsic exotic characteristics, introduction of magnetization into the topological insulator will modify the electronic. This exchange interaction between conduction electron and magnetic atoms breaks timereversal symmetry and that opens a gap of Dirac surface state. The Dirac fermion in the surface state becomes massive [1, 2, 21] and leads to many interesting properties, such as quantum anomalous Hall effect, [22, 23] topological magnetoelectric effect [24], tunability of chiral edge mode [25, 26] and Majorana braiding [27,28,29]. The carrier from the topological surface state dominates these magnetoelectrical properties. Many experimental works were performed in Mn, Cr, and Vdoped (Bi, Sb)\(_{2}\)Te\(_{3}\) thin films to realize the theoretical prediction [30]. Most of these studies mainly focused on electricmagneto transport properties, such as quantum anomalous Hall effect, topological magnetoelectric effect and related applications. Due to the weak magnetism signal in a thin film with weak magnetic elementdoped topological insulator, rare studies on the intrinsic magnetic properties of magnetdoped were reported in magnetic elementdoped topological insulators and the related magnetic coupling is not wellexplored. To understand the intrinsic novel physical properties of the magnetic element doped topological insulator, especially the role of the magnetic element and the related magnetic interaction coupling, it could be helpful to precisely utilize the magneto properties on the related application.
In this work, we studied the magnetic properties of Nidoped Sb\(_{2}\)Te\(_{3}\) topological insulator single crystal. A hysteresis loop with a low coercive field was observed below the Néel temperature (\(T_{\mathrm {N}}\)). The magnetic susceptibility reveals a kick at \(T_{\mathrm {N}}\) that is independent of the external magnetic field. The magnetic susceptibility of zero field cool and field cool processes coincide above \(T_{\mathrm {N}}\), and they are bifurcation below \(T_{\mathrm {N}}\). The magnetic susceptibility splitting is larger at lower external magnetic fields and temperatures. No more magnetic susceptibility splitting is observed at magnetic field above 7000 Oe. Our study supports that these magnetic susceptibility characteristics originates from an antiferromagnetic order accompanied by weak ferromagnetism. The extracted saturated susceptibility goes well with the tendency of the measured magnetic susceptibility cusp. Apart from most reports that the magnetic susceptibility cusp originates from the carrier spin texture at Dirac point of the topological surface state, our results reveal that it might be related to the ferromagnetism of magnetic elements.
Experimental Method
Single crystals of Sb\(_{2}\)Te\(_{3}\) were grown with a home made resistanceheated floating zone furnace (RHFZ). The starting raw materials of Sb\(_{2}\)Te\(_{3}\) were mixed according to the stoichiometric ratio. At first, the stoichiometric mixtures of high purity elements Ni (99.995%), Sb (99.995%) and Te (99.995%) were melted at \(700 \sim 800 ^{\circ }\)C for 20 h and then slowly cooled to room temperature in an evacuated quartz glass tube. The material was used as a feeding rod for the following RHFZ experiment. Our previous work supports that extremely high crystal uniformity in topological insulator crystals can be obtained through the RHFZ method. After growth, the crystals were then furnace cooled to room temperature. The asgrown crystals were cleaved along the basal plane, with a silvery shiny mirrorlike surface, and then prepared for further experiments. The Energydispersive spectrum (EDS) results support that the \(\mathrm {Ni} : \mathrm {Sb} : \mathrm {Te} = 0.017 : 2 : 3\). Figure 1 shows the Xray Diffraction (XRD) spectrum. It reveals sharp peaks and these peaks are consistent with the database of Sb\(_{2}\)Te\(_{3}\). This confirms that our sample is highly crystallized. The Ni atoms are expected to be uniformly and randomly distributed in the single crystal. The crystal size is 3mm long, 2mm wide and 0.42mm thickness. Magnetism measurements were performed using the standard technique in a commercial apparatus (Quantum Design MPMS) with a magnetic field of up to 7 T. The magnetic field was applied perpendicular to the large cleaved surface.
Results and Discussion
Figure 2 shows the magnetization as a function of magnetic fields at different temperatures, and it revealed the diamagnetic characteristic at a wide range of magnetic fields and temperatures. This diamagnetism comes from the carrier spin and it is consistent with the previous reports in BSTS topological insulators [31]. As shown in the topright inset, different from previous reports, a hysteresis loop was observed at temperatures below 125 K. The coercive field of the hysteresis loop shows weak temperature dependence and it is roughly 50 Oe. The remanent and saturated magnetization of the hysteresis loop is about \(10^{5}\) emu/g and \(10^{4}\) emu/g at 100 K. The low coercive field, the small remanent, and the small saturated magnetization indicate weak ferromagnetism. As shown in the bottomleft inset, no clear hysteresis loops were observed at temperatures above 125 K. The ferromagnetism originates from the aligned magnetic moments of the magnetic elements. The thermal energy might randomize the aligned magnetic moment and smear out the ferromagnetism above a critical temperature. Our observation indicates that the system reveals a weak ferromagnetism transition around 120 K.
To investigate the intrinsic magnetism characteristic of the observed weak ferromagnetic transition, the temperaturedependent magnetic susceptibility was performed through fieldcooled and zerofieldcooled processes. Figure 3 shows the magnetic susceptibility of fieldcooled and zerofield cooled processes at different external magnetic fields. The magnetic susceptibility increases as temperature decreases. It reveals a discontinuity at 125 K (\(T_{\mathrm {N}}\)) and the \(T_{\mathrm {N}}\) is independent of the external magnetic fields. The \(T_{\mathrm {N}}\) is the Néel temperature and the detailed mechanism will be discussed and clarified below. The magnetic susceptibility of fieldcooled and zerofieldcooled coincides above \(T_{\mathrm {N}}\) and bifurcates below \(T_{\mathrm {N}}\). A larger magnetic susceptibility splitting is observed at lower external magnetic fields. Our experimental result shows that this discontinuity and the magnetic susceptibility splitting is no more observed at magnetic field higher than 7000 Oe. It is worthy to notice that the signal fluctuation at the magnetic field of 50 Oe is obviously larger than other magnetic fields. One of the possible reasons is that the magnetic moment alignment is metastable at the 50 Oe that is close to the hysteresis loop coercive field. As shown in Fig. 2, the hysteresis loop was only observed below 125 K that is the same as the critical temperature of the magnetic susceptibility bifurcation in Fig. 3. This indicates the observed magnetic susceptibility splitting might be related to the weak ferromagnetic below the \(T_{\mathrm {N}}\). It is known that the ferromagnetic effect would be smeared out by thermal energy and the magnetic susceptibility above the critical temperature could be described by the CurieWeiss law, \(\chi = \chi _{0} + \frac{C}{T\theta }\), where \(\chi\) is the measured magnetic susceptibility, \(\chi _{0}\) is the magnetic susceptibility at 0 K, C is the Curie constant that is corresponding to the Bohr magneton, T is the temperature, and \(\theta\) is the Curie temperature [32]. The inset of Fig. 4 shows the temperature dependence of zerofield cooled \(\frac{1}{\chi  \chi _{0}}\) at different external magnetic fields. The \(\frac{1}{\chi \chi _{0}}\) is proportional to a temperature between 125 and 250 K, and the slope is larger at lower external magnetic fields. The slope is related to the Curie constant. The linear extrapolation of the \(\frac{1}{\chi \chi _{0}}\) between 125 and 250 K of all external magnetic fields coincide at 125 K. Following the CurieWeiss law, this value is corresponding to the \(\theta\). The negative \(\theta\) (125 K) indicates that it is an antiferromagnetic system below the \(T_{\mathrm {N}}\) and \(T_{\mathrm {N}}\) is known as Néel temperature [33]. The absolute value of the \(\theta\) is consistent with the observed \(T_{\mathrm {N}}\) in Fig. 3 , and the critical temperature to observe the hysteresis loop (125 K) in Fig. 2. These observations indicate that weak ferromagnetism and antiferromagnetism coexist below \(T_{\mathrm {N}}\).
As shown in the inset of Fig. 3, the Curie constant, C, is larger at higher magnetic fields. Following the Langevin paramagnetic function, C could be expressed as \(C=\frac{N\mu _{0}\mu ^{2}}{3k_{\mathrm {B}}T}\) where N is the number of magnetic elements per unit gram, \(\mu\) is the effective moment of a magnetic element, \(\mu _{0}\) is the vacuum permeability and \(k_{\mathrm {B}}\) is the Boltzmann constant [34]. The estimated \(\mu\) at 200 Oe is about 3.5 \(\mu _{\mathrm {B}}\) that is closed to the theoretical value of 3.32 \(\mu _{\mathrm {B}}\) [35]. This confirms that magnetism behavior could be explained by the CurieWeiss law.
The magnetic moment is randomly frozen in the zerofieldcool and frozen along the external magnetic field direction in the fieldcool. The magnetic susceptibility bifurcation originates from the magnetic anisotropy. This feature might be a characteristic for an antiferromagnetism order accompanied by weak ferromagnetism; ferromagnetic moments of domains freeze in a random direction in zerofieldcool, while they are forced to align along the applied magnetic field upon cooling across \(T_{\mathrm {N}}\) in field cool [36]. As discussed above, it composes of both weak ferromagnetic and antiferromagnetic characteristics below \(T_{\mathrm {N}}\) in our system. The weak ferromagnetic alignment would slightly break the antiferromagnetism order and induce the magnetic anisotropy. The magnetic susceptibility bifurcation could be understood as weak ferromagnetism in an antiferromagnetic system. These results support the observed magnetic susceptibility bifurcation below 125 K is the magnetic characteristic of the weak ferromagnetism in an antiferromagnetic system. The different susceptibility splitting at different external magnetic field might originate from the different partial polarization level of antiferromagnetism at external magnetic fields.
Following the mean field theory, [37] the \(T_{\mathrm {N}}\) is related to the exchange coupling strength, \(J_{0}\), and it could be expressed as \(T_{\mathrm {N}}=\frac{S(S+1)}{3k_{\mathrm {B}}T}J_{0}\), where S is the spin moment, \(k_{\mathrm {B}}\) is Boltzmann constant. The \(J_{0}\) would go to \(4.28 \times 10^{22}\) joule in our system with \(T_{\mathrm {N}}\) = 125 K. The mean field theory supports that the magnetization is related to the thermal energy by a factor of \(e^{\frac{J_{0}S}{k_{\mathrm {B}}T}}\). The magnetic susceptibility could be expressed as \(\chi = \chi _{\mathrm {S}}(1e^{\frac{J_{0}S}{k_{\mathrm {B}}T}})\), where \(\chi _{\mathrm {S}}\) is the saturated magnetic susceptibility. The magnetic susceptibility splitting, \(\chi _{\mathrm {FC}}\chi _{\mathrm {ZFC}}\) could be expressed as \(\chi _{\mathrm {S}}e^{\frac{J_{0}S}{k_{\mathrm {B}}T}}\). The \(\chi _{\mathrm {S}}\) is sensitive to external magnetic fields. As shown in the inset of Fig. 4, this equation could explain our experimental result well at a wide range of temperatures and external magnetic fields. The extracted \(\chi _{\mathrm {S}}\) is a function of external magnetic fields. To further examine the result, the magnetic field dependent susceptibility is performed at temperatures below \(T_{\mathrm {N}}\), and it shows a cusp at zero magnetic fields. This magnetic susceptibility cusp at zero magnetic field is widely observed in topological materials, and it is speculated to originate from the freealigned spin texture at the Dirac point [38]. The Angleresolved photoemission spectroscopy (ARPES) reveals that the Fermi level lies below the Dirac point in our Sb\(_{2}\)Te\(_{3}\) [39]. The observed cusp should not originate from the spin texture at the Dirac point. On the other hand, the coercive field of the hysteresis loop is about 50 Oe that is two orders of magnitude lower than full width at half maximum of the cusp, 0.4 T, and the hysteresis loop should not be the main source of the observed cusp. As shown in the inset of Fig. 4, the extracted magnetic fielddependent \(\chi _{\mathrm {S}}\) follows the same magnetic field tendency of the measured magnetic susceptibility. This indicates that the widely observed susceptibility cusp might originate from the antiferromagnetic order accompanied by weak ferromagnetism alignment.
Following the analysis, the susceptibility bifurcation originates from the magnetism of weak ferromagnetism order accompanied by antiferromagnetism. The magnetic susceptibility splitting is related to the magnetocrystalline anisotropy. Herewith, we further estimate the magnetocrystalline anisotropy energy, \(\Delta E = \frac{M_{\mathrm {S}}H_{\mathrm {C}}V}{2}\), where \(H_{\mathrm {C}}= 50\) Oe, \(M_{\mathrm {S}}= 1.81\times 10^{11}\) J/T and \(V=2.5\times 10^{9}\) m\(^{3}\) in our system, and the \(\Delta E \sim 1.13 \times 10^{22}\) Joule [40]. Following the magnetic moment energy, \(g\mu _{\mathrm {B}}B\), one could estimate that the magneto crystalline anisotropy energy will be lower than the magnetic moment energy at \(B > 0.61\) T. That is consistent with our observation that the magnetic susceptibility splitting is no longer observed at external magnetic fields above 0.7 T.
Figure 5 shows the magnetic susceptibility as a function of 1/B and it shows periodic oscillations. This is known as the De HaasVan Alphen effect (dHvA) oscillations that originate from the orbital motion of itinerant electron at high magnetic fields [41]. We analyze the dHvA oscillations by fitting the oscillatory magnetization to the LifshitzKosevich (LK) formula [42], \(\Delta M \propto R \sin [2\pi (\frac{F}{B}\delta _{p})]\). R is related to the carrier scattering rate, Zeeman effect, and Landau level broadening [43]. The oscillation is described by a sinusoidal term that contains the phase factor \(\delta _{p}\). \(\delta _{p}\) is related to the Berry phase (\(\Phi _{B}\)), \(\delta _{p} = \frac{1}{2}\frac{\Phi _{B}}{2\pi }\). The dimension of the Fermi pocket characterizes the value \(\delta _{p}\). As shown in Fig. 5, the theoretical equation fits well with our experimental result and the extracted \(\delta _{p}=0.43\) and \(F = 29.8\) T. That is consistent with the theoretical prediction and the observed dHvA comes from the topological surface state. Following the Onsager relation [44], \(F=\frac{\hbar K_F^{2}}{2\pi }\), one could estimate that \(K_{F} = 0.030\)Å^{−}^{1} is consistent with the reported value from ARPES. These results suggest that the dHvA oscillations originate from the topological surface state.
Conclusion
In this work, we studied the magnetic behavior of Nidoped Sb\(_{2}\)Te\(_{3}\) topological insulator single crystal. A hysteresis loop with low a coercive field was observed below the Néel temperature. The magnetic susceptibility reveals a kick at Nèel temperature that is independent of the external magnetic field. The magnetic susceptibility of zero field cool and field cool processes are coinciding above the Néel temperature, and they are bifurcation below Néel temperature. The magnetic susceptibility splitting is larger at a lower external magnetic field. No more magnetic susceptibility splitting is observed when the magnetic moment anisotropy energy is lower than the magnetic moment energy at 0.7 T. Our study supports that these magnetic susceptibility characteristics originate from an antiferromagnetic order accompanied by weak ferromagnetism. The extracted saturated magnetic susceptibility goes well with the tendency of the measured magnetic susceptibility cusp. This indicates that the widely observed susceptibility cusp might originate from the weak ferromagnetism. The dHvA oscillation is consistent with the theoretical prediction. This supports that observed dHvA oscillation comes from the topological surface state.
Availability of data and materials
The datasets generated during and/or analyzed during the current study are available from the corresponding authors on reasonable request.
Abbreviations
 XPD:

Xray diffraction
 EDS:

Energydispersive Xray spectroscopy
 ARPES:

Angle resolved photoemission spectroscopy
 dHvA:

De HaasVan Alphen
References
 1.
Hasan MZ, Kane CL (2010) Topological insulators. Rev Mod Phys 82:3045–3067
 2.
Qi XL, Zhang SC (2011) Topological insulators and superconductors. Rev Mod Phys 83:1057–1110
 3.
Leek PJ et al (2007) Observation of Berry’s phase in a solidstate qubit. Science 318:1889–1892
 4.
Fu L, Kane CL (2008) Superconducting proximity effect and majorana fermions at the surface of a topological insulator. Phys Rev Lett 100:0964071096407–4
 5.
Wolf SA et al (2001) A spinbased electronics vision for the future. Science 294:1488–1495
 6.
Neupane M et al (2014) Observation of quantumtunnelling modulated spin texture in ultrathin topological insulator Bi2Se3 films. Nat Commun 5:38411–38417
 7.
Pan ZH et al (2011) Electronic structure of the topological insulator Bi2Se3 using angleresolved photoemission spectroscopy: evidence for a nearly full surface spin polarization. Phys Rev Lett 106:2570041–2570044
 8.
Li CH et al (2014) Electrical detection of chargecurrentinduced spin polarization due to spinmomentum locking in Bi_{2}Se_{3}. Nat Nanotechnol 9:218–224
 9.
Ando Y et al (2014) Electrical detection of the spin polarization due to charge flow in the surface state of the topological insulator Bi_{1.5}Sb_{0.5}Te_{1.7}Se_{1.3}. Nano Lett 14, 62266230
 10.
Tang JS et al (2014) Electrical detection of spinpolarized surface states conduction in (Bi_{0.53}Sb_{0.47})_{2}Te_{3} topological insulator. Nano Lett 14, 54235429
 11.
Mellnik AR et al (2014) Spintransfer torque generated by a topological insulator. Nature 511:449–451
 12.
Deorati P et al (2014) Observation of inverse spin Hall effect in bismuth selenide, Phys Rev B 90, 09440310944036
 13.
Shiomi Y et al (2014) Spinelectricity conversion induced by spin injection into topological insulators. Phys Rev Lett 113:1966011196601–5
 14.
Baker AA, Figueroa AI, CollinsMcIntyre LJ, vander Laan G, Hesjedala T (2015) Spin pumping in ferromagnettopological insulatorferromagnet heterostructures. Sci Rep 5:79071–79075
 15.
Yan Y et al (2014) Topological surface state enhanced photo thermoelectric effect in Bi_{2}Se_{3} nanoribbons. Nano Lett 14:4389–4394
 16.
Yan Y, Wang LX, Yu DP, Liao ZM (2013) Large magnetoresistance in high mobility topological insulator Bi_{2}Se_{3}. Appl Phys Lett 103:0331061–0331064
 17.
Yan Y et al (2013) Synthesis and quantum transport properties of Bi_{2}Se_{3} topological insulator nanostructures. Sci Rep 3:12641–12645
 18.
Yan Y et al (2014) Highmobility Bi_{2}Se_{3} nanoplates manifesting quantum oscillations of surface states in the sidewalls. Sci Rep 4:38171–38177
 19.
Li X et al (2019) Spinresolved electronic and transport properties of graphynebased nanojunctions with different Nsubstituting positions. Nanoscale Res Lett 14, 2991–29912
 20.
Li X et al (2018) Spincharge transport properties of a Zshaped αgraphyne nanoribbon junction with different edge passivations. Carbon 131:160–167
 21.
Tokura Y, Yasuda K, Tsukazaki A (2019) Magnetic topological insulators. Nat Rev Phys 1:126–143
 22.
Chang CZ et al (2013) Experimental observation of the quantum anomalous Hall effect in a magnetic topological insulator. Science 340:167–170
 23.
Liu CX, Zhang SC, Qi XL (2016) The quantum anomalous Hall effect: theory and experiment. Ann Rev Condens Matter Phys 7:301–321
 24.
Dziom V et al (2017) Observation of the universal magnetoelectric effect in a 3D topological insulator. Nat Commun 8:1–8
 25.
Yasuda K et al (2017) Quantized chiral edge conduction on domain walls of a magnetic topological insulator. Science 358:1311–1314
 26.
Ilan RT et al (2017) Chiral transport along magnetic domain walls in the quantum anomalous Hall effect. NPJ Quantum Mater 2:1–6
 27.
Fu L, Kane CL (2008) Superconducting proximity effect and majorana fermions at the surface of a topological insulator. Phys Rev Lett 100:096407
 28.
Wilczek F (2009) Majorana returns. Nat Phys 5:614–618
 29.
Alicea J (2012) New directions in the pursuit of Majorana fermions in solid state systems. Rep Prog Phys 75:076501
 30.
Lee JS et al (2014) Ferromagnetism and spindependent transport in ntype Mndoped bismuth telluride thin films. Phys Rev B 89:174425
 31.
Zyuzin AA, Hook MD, Burkov AA (2011) Parallel magnetic field driven quantum phase transition in a thin topological insulator film. Phys Rev B 83:245428
 32.
Irfan B, Chatterjee R (2015) Magnetotransport and Kondo effect in cobalt doped Bi_{2}Se_{3} topological insulators. Appl Phys Lett 107:173108
 33.
Takahashi T (1986) On the origin of the CurieWeiss law of the magnetic susceptibility in itinerant electron ferromagnetism. J Phys Soc Jpn 55:3553–3573
 34.
Amaladass EP et al (2019) Studies on Shubnikovde Haas oscillations and magnetic properties of cobaltdoped Bi_{1.9}Co_{0.05}Sb_{0.05}Se_{3} topological single crystals. J Alloys Comps 775:1094–1100
 35.
Larson P, Lambrecht WR (2008) Electronic structure and magnetism in Bi_{2}Te_{3}, Bi_{2}Se_{3}, and Sb_{2}Te_{3} doped with transition metals (TiZn). Phys Rev B 78:195207
 36.
Vogl M et al (2020) Complex magnetic properties in the mixed 4f–5d double perovskite iridates X_{2}ZnIrO_{6} (X = Nd, Sm, Eu, Gd). Phys Rev Mater 4:054413
 37.
Negele JW (1982) The meanfield theory of nuclear structure and dynamics. Rev Mod Phys 54:913
 38.
Zhao L et al (2014) Singular robust roomtemperature spin response from topological Dirac fermions. Nat Mater 13:580–585
 39.
Zhu S et al (2015) Ultrafast electron dynamics at the Dirac node of the topological insulator Sb_{2}Te_{3}. Sci Rep 5:1–6
 40.
Meiklejohn WH, Bean CP (1956) New magnetic anisotropy. Phys Rev 102:1413
 41.
Taskin AA, Ando Y (2009) Quantum oscillations in a topological insulator Bi_{1−x}Sb_{x}. Phys Rev B 80:085303
 42.
Peschanskii VG, Yu Kolesnichenko A (2014) On the 60th anniversary of the Lifshitz–Kosevich theory. Low Temp Phys 40:267–269
 43.
Hu J et al (2016) Evidence of topological nodalline fermions in ZrSiSe and ZrSiTe. Phys Rev Lett 117:016602
 44.
Zhi Ren AA (2010) Taskin, Satoshi Sasaki, Kouji Segawa, and Yoichi Ando, Large bulk resistivity and surface quantum oscillations in the topological insulator Bi_{2}Te_{2}Se. Phys Rev B 82:241306(R)
Funding
This work was supported by the Ministry of Science and Technology, Taiwan through Grant No. 1072112M110011MY2, 1082918I110007, 1092112M110018, 1102112M110021, and Center of Crystal Research at National Sun YatSen University. Service plan of corefacility center at NSYSU through MOST1102731M110001, MOST1082731M110001, MOST1072731M110001, and MOST1062731M110001 SMH thanks the support of shortterm oversea reserach project for scientist and technician from the Taiwan National Science Council.
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SMH conceive the idea, analysis these experimental results and prepare the paper. PCW analyzed the data. HLJ and M.M.C.C. grow the high quality crystal. All authors reviewed the manuscript. All authors read approved the final manuscript.
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Huang, SM., Wang, PC., Jian, HL. et al. The Magnetic Susceptibility Bifurcation in the NiDoped Sb_{2}Te_{3} Topological Insulator with Antiferromagnetic Order Accompanied by Weak Ferromagnetic Alignment. Nanoscale Res Lett 16, 180 (2021). https://doi.org/10.1186/s11671021036375
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DOI: https://doi.org/10.1186/s11671021036375
Keywords
 Antiferromagnetism
 Ferromagnetism topological material
 Magnetic susceptibility
 Curie–Weiss law