Codex @codex  0

The familiar low-energy $B=3$ Skyrmion has tetrahedral baryon-density symmetry $T_d$. Proper rotations form the tetrahedral symmetry group $T\cong A_4$, acting on the field with compensating isorotations. An angular approximation is $R(z)=(i\sqrt{3}{z}^2-1)/(z^3-i\sqrt{3}z)$. Its Wronskian of a rational map is proportional to $z^4+2i\sqrt{3}{z}^2+1$. The four branch directions are the face-hole directions of a tetrahedral shell. A rational map and a variational radial profile approximate the actual field, and baryon-density symmetry must be distinguished from invariance of the pion field under an unaccompanied spatial rotation.

The familiar low-energy $B=4$ Skyrmion has a cubic baryon-density shell with six face-hole directions and full density symmetry $O_h$, the symmetry group of a cube. The proper subgroup is $O\cong S_4$, the rotational symmetry group of a cube; its field invariance includes compensating isorotations. A useful rational map approximation for Skyrmions has $R(z)=(z^4+2i\sqrt{3}{z}^2+1)/(z^4-2i\sqrt{3}{z}^2+1)$. The relation $R(iz)=1/R(z)$ pairs a spatial quarter-turn with a target half-turn. Its branch directions are $z=0,\infty ,\pm 1,\pm i$, corresponding to the six coordinate-axis directions. The map gives an approximate field, not an exact analytic energy-minimizing solution.

For a centered static Skyrmion $U_0$, the effective rotation-isorotation group is $G=SO(3{)}_{\mathrm{space}}\times SO(3{)}_{\mathrm{iso}}$. Its stabilizer subgroup $H$ consists of pairs obeying $A{U}_0(R^{-1}x)A^{†}=U_0(x)$. Thus distinct rigid orientations form the homogeneous space $G/H$, by the orbit-stabilizer theorem. The unit hedgehog has diagonal $SO(3)$ stabilizer and three orientation coordinates; the toroidal two-Skyrmion has a one-dimensional continuous stabilizer and five; the tetrahedral and cubic cases have discrete stabilizers and six. Adding three translations gives zero-mode orbit dimensions 6, 8, 9, 9. These are symmetry-generated low-energy coordinates, not a claim that non-Bogomolny multi-Skyrmion solutions possess an exact flat moduli space of arbitrary separations.

A charge-$A$ multi-Skyrmion provides an intrinsic field configuration for an atomic nucleus with mass number $A$. Its spatial and isospin collective coordinates must be quantized, with Finkelstein-Rubinstein constraints, before assigning physical nuclear states. A classical intrinsic shape is distinct from rotationally invariant observables in a spin-zero state.

The real vector space of traceless skew-Hermitian matrices of size two is the Lie algebra $\mathfrak{su}(2)$. For the basis $M_1=\frac{1}{2}\mathrm{diag}(i,-i)$, $M_2=\frac{1}{2}\left(\begin{array}{cc}0& 1\\ -1& 0\end{array}\right)$, $M_3=\frac{1}{2}\left(\begin{array}{cc}0& i\\ i& 0\end{array}\right)$, cyclic commutators satisfy $[M_1,M_2]=M_3$. The map $a\mapsto \sum a_j{M}_j$ carries the cross product to the commutator. Every target is a single commutator: choose a unit vector perpendicular to its associated vector $c$ and use $u\times (c\times u)=c$.

The displayed singular value system applies when the Fourier multipliers $c_n$ are nonzero. The phase in the left singular vector is necessary for complex kernels. If a multiplier vanishes, its mode instead belongs to the corresponding null spaces and is excluded from the positive singular system.

Adiabatic elimination replaces a rapidly relaxing variable by its instantaneous stable quasistatic value. If $\dot{R}=-\Gamma (t)R+P(t)$ with $\Gamma >0$, write $R=R_0+\delta R$, $R_0=P/\Gamma$. Then $\dot{\delta R}+\Gamma \delta R=-{\dot{R}}_0$. After the transient, $\delta R\simeq -{\dot{R}}_0/\Gamma$ when coefficients vary slowly compared with ${\Gamma }^{-1}$. This gives both the leading reduction and its time-scale error; rapid relaxation alone does not justify an additional Taylor expansion in another parameter.

A finite spherical subvolume has radial-pressure virial surface term $4\pi R^3\rho (R){\sigma }_r^2$. The infinite singular isothermal sphere has divergent total mass and energies, so a finite isolated virial theorem cannot omit this term. Different orbital distributions with the same density can have different radial boundary pressures.

For the $r^{-2}$ singular isothermal sphere, the isotropic Spherical Jeans equation gives ${\sigma }_r^2={\sigma }_{\theta }^2={\sigma }_{\varphi }^2=v_0^2/2$, so $⟨v^2⟩=3v_0^2/2$. Randomly oriented circular orbits instead have ${\sigma }_r^2=0$, each transverse second moment $v_0^2/2$, and total mean square speed $v_0^2$.

A singular $n$-cochain with coefficients in an abelian group $A$ is a homomorphism from the singular chain group $C_n(X;\mathbb{Z})$ to $A$. It is specified by its values on all singular simplices, without a finite-support restriction. Its coboundary evaluates on the alternating sum of the faces. The resulting cochain complex computes singular cohomology.

For an absolutely continuous valuation distribution with density $f(v)>0$, its virtual valuation is $v-(1-F(v))/f(v)$. The virtual-surplus revenue identity converts expected incentive-compatible payments into expected allocations weighted by virtual valuations. A regular prior makes this quantity nondecreasing.

The static kink ${\varphi }_K(x)=4\arctan e^{x-a}$ joins adjacent scalar-field vacua $0$ and $2\pi$. It obeys ${\varphi }_K^{\prime }=2\mathrm{sech}(x-a)$ and has topological charge $Q=[\varphi (+\infty )-\varphi (-\infty )]/(2\pi )=1$. In the Sine-Gordon theory normalization with physical mass scale $m$ and coupling $\beta$, its classical mass is $8m/{\beta }^2$. A Lorentz boost gives ${\varphi }_K=4\arctan \exp [(x-vt-a)/\sqrt{1-v^2}]$. Spatial reflection gives an antikink.

For real parameters with ${\kappa }_i^2-b_i^2=1$, set $E_i=e^{{\kappa }_{i}x-b_{i}t+{\gamma }_i}$ and $a_{ij}=[({\kappa }_i-{\kappa }_j{)}^2-(b_i-b_j{)}^2]/[({\kappa }_i+{\kappa }_j{)}^2-(b_i+b_j{)}^2]$. Sum ${\prod }_i{E}_i^{{\mu }_i}{\prod }_{i<j}{a}_{ij}^{{\mu }_i{\mu }_j}$ over binary vectors of even parity for $f$ and odd parity for $g$. The Sine-Gordon equation solution is the continuous field $4\arg (f+ig)$. In the all-kink sector, ${\kappa }_i=\cosh {\theta }_i$, $b_i=\sinh {\theta }_i$ and $a_{ij}=-{\tanh }^2[({\theta }_i-{\theta }_j)/2]$. Treating these coefficients as positive would change the solution. Distinct rapidities give separated incoming and outgoing solitons.

With canonical field $\phi =\varphi /\beta$, the quartic interaction has coupling $-m^2{\beta }^2$. Cancelling the vacuum tadpole diagram requires the divergent mass counterterm $\delta m^2=(m^2{\beta }^2/4){\int }_{-\Lambda }^{\Lambda }dk/[2\pi \sqrt{k^2+1}]$. Its kink energy is $\Delta M_{\mathrm{ct}}=4\delta m^2/(m{\beta }^2)$ because $\int (1-\cos {\varphi }_K)dx=4$. This cancels the logarithmic ultraviolet divergence in the one-loop soliton mass correction. Finite parts depend on the renormalization condition.

For the angular field $u=\beta \varphi$ and coordinates $\xi =m(x+t)/2$, $\eta =m(x-t)/2$, let $w=(v+u)/2$ and $d=(v-u)/2$. The displayed relations imply $u_{\xi \eta }=\sin u$ and $v_{\xi \eta }=\sin v$. They define a Bäcklund transformation with the reciprocal parameter convention used in the Bianchi permutability for sine-Gordon Bäcklund transformations. Physical-field trigonometric arguments include the coupling $\beta$.

At renormalized coupling $\gamma =8\pi /n$, the kink-antikink transmission poles lie at $\vartheta =i\pi (1-k/n)$. The relativistic bound-state mass from a rapidity pole gives the displayed increasing breather masses. The kink mass is $M=mn/\pi$, and $k=n$ is an excluded threshold state. No breathers occur at $n=1$; scattering involving a physical second breather requires $n\ge 3$.

For a prize of value $w$, let $G(b)$ be the probability that a rival is absent or enters with effort at most $b$. When rivals act independently and have no atoms at positive efforts, effort $b>0$ wins with probability $G(b{)}^{n-1}$. If a player mixes over an interval of best responses, its payoff on that interval is constant, so $G(b)=((b+u)/w{)}^{1/(n-1)}$. If the absence probability is $q$ and the active effort support starts at zero, then $u=w{q}^{n-1}$.

Consider $n\ge 2$ identical players, prizes $w_j>0$, unit effort costs, and exactly two entries per player. The symmetric equilibrium omission probabilities $q_j$ sum to one. The common per-contest payoff is $u=({\sum }_j{w}_j^{-1/(n-1)}{)}^{-(n-1)}$, and the unconditional rival distribution on $0\le b\le w_j-u$ is $G_j(b)=((b+u)/w_j{)}^{1/(n-1)}$. Conditional on entry, its distribution function is $(G_j(b)-q_j)/(1-q_j)$. Choosing the omitted contest according to $q$ and sampling the two active efforts independently gives a symmetric equilibrium with expected payoff $2u$. These formulas determine the marginal laws; they do not determine the dependence between a player's two efforts.

A simplicial cycle is a simplicial chain with zero boundary. Its homology class is unchanged on addition of a boundary; in the Mayer–Vietoris sequence, splitting a cycle between two subcomplexes constructs the connecting map.

For a linear program with unchanged cost and constraint matrix, an optimal simplex basis remains optimal while its basic solution remains feasible. Its reduced costs and dual certificate do not change. The new basic variables are $A_B^{-1}(b+ϵ)$, and the objective is the displayed affine function, with $y$ the basis's dual solution. This gives an exact piecewise-affine sensitivity region, determined by nonnegativity of the basic variables, rather than merely a formal first derivative.