Skyrmion

In field theory, skyrmions are homotopically non-trivial classical solutions of a nonlinear sigma model^[17] with a non-trivial target manifold topology – hence, they are topological solitons. An example occurs in chiral models^[18] of mesons, where the target manifold is a homogeneous space of the structure group

${\displaystyle \left({\frac {\operatorname {SU} (N)_{L}\times \operatorname {SU} (N)_{R}}{\operatorname {SU} (N)_{\text{diag}}}}\right),}$ 

where SU(N)_L and SU(N)_R are the left and right chiral symmetries, and SU(N)_diag is the diagonal subgroup. In nuclear physics, for N = 2, the chiral symmetries are understood to be the isospin symmetry of the nucleon. For N = 3, the isoflavor symmetry between the up, down and strange quarks is more broken, and the skyrmion models are less successful or accurate.

If spacetime has the topology S³×R, then classical configurations can be classified by an integral winding number^[19] because the third homotopy group

${\displaystyle \pi _{3}\left({\frac {\operatorname {SU} (N)_{L}\times \operatorname {SU} (N)_{R}}{\operatorname {SU} (N)_{\text{diag}}}}\cong \operatorname {SU} (N)\right)}$ 

is equivalent to the ring of integers, with the congruence sign referring to homeomorphism.

A topological term can be added to the chiral Lagrangian, whose integral depends only upon the homotopy class; this results in superselection sectors in the quantised model. In (1 + 1)-dimensional spacetime, a skyrmion can be approximated by a soliton of the Sine–Gordon equation; after quantisation by the Bethe ansatz or otherwise, it turns into a fermion interacting according to the massive Thirring model.

The Lagrangian for the skyrmion, as written for the original chiral SU(2) effective Lagrangian of the nucleon-nucleon interaction (in (3 + 1)-dimensional spacetime), can be written as

${\displaystyle {\mathcal {L}}={\frac {-f_{\pi }^{2}}{4}}\operatorname {tr} (L_{\mu }L^{\mu })+{\frac {1}{32g^{2}}}\operatorname {tr} [L_{\mu },L_{\nu }][L^{\mu },L^{\nu }],}$ 

where ${\displaystyle L_{\mu }=U^{\dagger }\partial _{\mu }U}$ , ${\displaystyle U=\exp i{\vec {\tau }}\cdot {\vec {\theta }}}$ , ${\displaystyle {\vec {\tau }}}$  are the isospin Pauli matrices, ${\displaystyle [\cdot ,\cdot ]}$  is the Lie bracket commutator, and tr is the matrix trace. The meson field (pion field, up to a dimensional factor) at spacetime coordinate ${\displaystyle x}$  is given by ${\displaystyle {\vec {\theta }}={\vec {\theta }}(x)}$ . A broad review of the geometric interpretation of ${\displaystyle L_{\mu }}$  is presented in the article on sigma models.

When written this way, the ${\displaystyle U}$  is clearly an element of the Lie group SU(2), and ${\displaystyle {\vec {\theta }}}$  an element of the Lie algebra su(2). The pion field can be understood abstractly to be a section of the tangent bundle of the principal fiber bundle of SU(2) over spacetime. This abstract interpretation is characteristic of all non-linear sigma models.

The first term, ${\displaystyle \operatorname {tr} (L_{\mu }L^{\mu })}$  is just an unusual way of writing the quadratic term of the non-linear sigma model; it reduces to ${\displaystyle -\operatorname {tr} (\partial _{\mu }U^{\dagger }\partial ^{\mu }U)}$ . When used as a model of the nucleon, one writes

${\displaystyle U={\frac {1}{f_{\pi }}}(\sigma +i{\vec {\tau }}\cdot {\vec {\pi }}),}$ 

with the dimensional factor of ${\displaystyle f_{\pi }}$  being the pion decay constant. (In 1 + 1 dimensions, this constant is not dimensional and can thus be absorbed into the field definition.)

The second term establishes the characteristic size of the lowest-energy soliton solution; it determines the effective radius of the soliton. As a model of the nucleon, it is normally adjusted so as to give the correct radius for the proton; once this is done, other low-energy properties of the nucleon are automatically fixed, to within about 30% accuracy. It is this result, of tying together what would otherwise be independent parameters, and doing so fairly accurately, that makes the Skyrme model of the nucleon so appealing and interesting. Thus, for example, constant ${\displaystyle g}$  in the quartic term is interpreted as the vector-pion coupling ρ–π–π between the rho meson (the nuclear vector meson) and the pion; the skyrmion relates the value of this constant to the baryon radius.

The local winding number density (or topological charge density) is given by

${\displaystyle {\mathcal {B}}^{\mu }=\epsilon ^{\mu \nu \alpha \beta }\operatorname {Tr} \{L_{\nu }L_{\alpha }L_{\beta }\},}$ 

where ${\displaystyle \epsilon ^{\mu \nu \alpha \beta }}$  is the totally antisymmetric Levi-Civita symbol (equivalently, the Hodge star, in this context).

As a physical quantity, this can be interpreted as the baryon current; it is conserved: ${\displaystyle \partial _{\mu }{\mathcal {B}}^{\mu }=0}$ , and the conservation follows as a Noether current for the chiral symmetry.

The corresponding charge is the baryon number:

${\displaystyle B=\int d^{3}x\,{\mathcal {B}}^{0}(x).}$ 

Which is conserved due to topological reasons and it is always an integer. For this reason, it is associated with the baryon number of the nucleus. As a conserved charge, it is time-independent: ${\displaystyle dB/dt=0}$ , the physical interpretation of which is that protons do not decay.

In the chiral bag model, one cuts a hole out of the center and fills it with quarks. Despite this obvious "hackery", the total baryon number is conserved: the missing charge from the hole is exactly compensated by the spectral asymmetry of the vacuum fermions inside the bag.^[20][21][22]

One particular form of skyrmions is magnetic skyrmions, found in magnetic materials that exhibit spiral magnetism due to the Dzyaloshinskii–Moriya interaction, double-exchange mechanism^[23] or competing Heisenberg exchange interactions.^[24] They form "domains" as small as 1 nm (e.g. in Fe on Ir(111)).^[25] The small size and low energy consumption of magnetic skyrmions make them a good candidate for future data-storage solutions and other spintronics devices.^[26][27][28] Researchers could read and write skyrmions using scanning tunneling microscopy.^[29][30] The topological charge, representing the existence and non-existence of skyrmions, can represent the bit states "1" and "0". Room-temperature skyrmions were reported.^[31][32]

Skyrmions operate at current densities that are several orders of magnitude weaker than conventional magnetic devices. In 2015 a practical way to create and access magnetic skyrmions under ambient room-temperature conditions was announced. The device used arrays of magnetized cobalt disks as artificial Bloch skyrmion lattices atop a thin film of cobalt and palladium. Asymmetric magnetic nanodots were patterned with controlled circularity on an underlayer with perpendicular magnetic anisotropy (PMA). Polarity is controlled by a tailored magnetic-field sequence and demonstrated in magnetometry measurements. The vortex structure is imprinted into the underlayer's interfacial region by suppressing the PMA by a critical ion-irradiation step. The lattices are identified with polarized neutron reflectometry and have been confirmed by magnetoresistance measurements.^[33][34]

A recent (2019) study^[35] demonstrated a way to move skyrmions, purely using electric field (in the absence of electric current). The authors used Co/Ni multilayers with a thickness slope and Dzyaloshinskii–Moriya interaction and demonstrated skyrmions. They showed that the displacement and velocity depended directly on the applied voltage.^[36]

In 2020, a team of researchers from the Swiss Federal Laboratories for Materials Science and Technology (Empa) has succeeded for the first time in producing a tunable multilayer system in which two different types of skyrmions – the future bits for "0" and "1" – can exist at room temperature.^[37]

• Hopfion, 3D counterpart of skyrmions

• Developments in Magnetic Skyrmions Come in Bunches, IEEE Spectrum 2015 web article
• Manton, N. (2022). Skyrmions - A Theory of Nuclei. World Scientific. ISBN 978-1800612471.