A symmetric stable distribution has this characteristic function, with $c>0$ and location $\mu$. At location zero it is a strictly stable distribution: weighted sums of independent copies have scale factor $({\sum }_j|a_j{|}^{\alpha }{)}^{1/\alpha }$. The index $\alpha$ need not permit a finite mean or variance. The scale in this convention is $c^{1/\alpha }$, so the coefficient of $|t{|}^{\alpha }$ and the scale parameter should not be confused.

Equating an inertial eddy turnover time to the inverse buoyancy frequency gives the scale separating buoyancy-affected motions from a smaller approximately isotropic cascade. It is distinct from the viscous Kolmogorov microscales. In very stable local surface-layer scaling it is proportional to the Obukhov length, up to closure constants.

For cellular Omega-spectra $D,E$, natural degree-preserving additive operations $D^{\ast }\to E^{\ast }$ commuting with suspension are compatible families $[D_j,E_j{]}_{\ast }$ by the Yoneda lemma. Since $D\simeq {\mathrm{hocolim}}_j{\Sigma }^{-j}{\Sigma }^{\infty }{D}_j$, the Milnor exact sequence for maps of spectra realizes every such family. Its kernel consists precisely of hyperphantom maps of spectra. Thus operations determine stable maps only modulo that kernel.

The weak stable bundle adjoins the flow direction to the strong stable bundle. It is tangent to the weak stable foliation. For a geodesic flow on a hyperbolic surface, the canonical frame gives $E^{ws}=\mathrm{span}\{X,H-V\}$.

For real base-flow velocity and positive Reynolds number, multiply the homogeneous Squire equation by the conjugate mode and integrate with zero endpoint values. Taking real parts gives the displayed negative temporal growth rate. This proves decay of homogeneous Squire modes; the coupled shear-flow system can still be unstable or show transient growth because wall-normal velocity can force the Squire variable.

Exchanging a down-type squark of mass $M$ between $LQD$ and $UDD$ vertices produces a dimension-six effective operator with coefficient $C\sim {\lambda }^{\prime }{\lambda }^{\prime \prime }/M^2$. Dimensional analysis then gives a proton decay width ${\Gamma }_p=c_h|{\lambda }^{\prime }{\lambda }^{\prime \prime }{|}^2{m}_p^5/M^4$, with a dimensionless factor $c_h$ containing hadronic matrix elements and phase space. A lifetime bound ${\tau }_p>{\tau }_{\min }$ implies $|{\lambda }^{\prime }{\lambda }^{\prime \prime }|<M^2/\sqrt{c_h{\tau }_{\min }{m}_p^5}$. The bound is on the relevant flavour product and depends on the exchanged mass; dimensional analysis alone does not determine $c_h$.

The R-parity violation vertices from $LQD$ and $UDD$ can both contain the same down-type squark. Write its linear couplings as $-\tilde{d}A-{\tilde{d}}^{\ast }{A}^{†}$ and its mass term as $-M^2|\tilde{d}{|}^2$. Eliminating it gives $A^{†}A/M^2$. The cross term is $({\lambda }^{\prime }{\lambda }^{\prime \prime \ast }/M^2)(\nu d_L-e{u}_L)(u^{c†}{d}^{c†})+h.c.$, with the color Levi-Civita symbol contracting the three quarks. It changes baryon number and lepton number together and supplies the dimension-six proton-decay operator for $p\to e^{+}{\pi }^0$. The two down-flavor indices in $UDD$ must differ, so strange- or bottom-squark exchange is allowed but identical down flavors vanish.

A scalar mode that changes sign under a quarter-turn and is fixed by diagonal reflections couples quadratically through $AC,BC,A^2-B^2$. In the saturated three-mode equivariant dynamical system, a diagonal state $A=B=s$, $C=0$ has $s^2={\mu }_1/(1+\lambda )$ and $p=2(\lambda -1)s^2$. The symmetric perturbation decays at rate $2{\mu }_1$; the remaining stability matrix is the displayed block. With $K=2{\alpha }_1{\gamma }_1/(\lambda -1)>0$, its linear stability interval is $-K<{\mu }_2<-p$, provided $p<K$. The endpoints are a symmetry-breaking pitchfork bifurcation and a Hopf bifurcation, respectively, away from degeneracies.

For the four wavevectors $(2,1),(2,-1),(1,2),(1,-2)$ and their negatives, use invariant phases ${\chi }_1=2{\theta }_1-2{\theta }_2-{\theta }_3+{\theta }_4$, ${\chi }_2={\theta }_1+{\theta }_2-2{\theta }_3-2{\theta }_4$. Add to the cubic normal form of a dynamical system the two quintic terms $e{\overline{A}}_2{A}_3^2{A}_4^2$ and $f{\overline{A}}_1{A}_2^2{A}_3{\overline{A}}_4$ in the first equation, together with their square-symmetry partners; $e,f$ are real. For equal positive magnitudes, steadiness forces $\sin {\chi }_1=\sin {\chi }_2=0$ unless $e=f=0$. Equality of radial equations further gives $(e-f)(\cos {\chi }_1-\cos {\chi }_2)=0$. Consequently the generic phase types are $(0,0)$ and $(\pi ,\pi )$. When $e=f\ne 0$, the mixed type $(0,\pi )$, equivalent by square symmetry to $(\pi ,0)$, also exists. When both quintic coefficients vanish, every phase pair is allowed. Amplitude existence must still be checked from the remaining scalar equation.

For a square-root stock claim priced by $C(t,T)=\mathbb{E}[\sqrt{S_T}\mid {\mathcal{F}}_t]$, the constant-volatility geometric Brownian motion price is $\sqrt{S_t}\exp (-{\sigma }^2(T-t)/8)$. If $t<T$, $S_t>0$ and $0<C(t,T)\le \sqrt{S_t}$, its unique nonnegative inverse volatility is the displayed $\Sigma (t,T)$. For bounded predictable volatility in $dS=S\sigma dW$, bounds $0\le a\le \sigma \le b$ give $a\le \Sigma \le b$, without independence from the Brownian motion. At zero stock price the claim price is also zero and no volatility is identified by this equation; a separate convention is needed.

For a finite extension $K/{\mathbb{Q}}_p$, its square-class group of a field is $K^{\times }/(K^{\times }{)}^2$. When $p$ is odd, parity of the valuation and the square class of the unit residue give $C_2\times C_2$. Representatives are $1,u,\pi ,u\pi$, where $\pi$ is a uniformizer of $K$ and $u$ has nonsquare residue. The Hensel lemma lifts square roots of units with square residue.

For $K={\mathbb{Q}}_2$, the group is $C_2^3$, with generators $-1,5,2$; a unit is a square exactly when it is one modulo eight. More generally, if $K/{\mathbb{Q}}_2$ has degree $d$, the group has order $2^{d+2}$. Indeed, the principal-unit group of a mixed-characteristic local field has a finite cyclic 2-power torsion factor and a free ${\mathbb{Z}}_2$ factor of rank $d$, each contributing its quotient by squares, and the valuation contributes one further factor $C_2$. The specific representatives $1,u,p,up$ therefore apply to ${\mathbb{Q}}_p$ for odd $p$; a ramified extension needs its own uniformizer.

The spring constant is the positive proportionality coefficient in the ideal spring restoring force $F=-kx$. Its SI unit is newtons per metre. With a constant attached mass $m$, it sets the angular frequency $\omega =\sqrt{k/m}$ of simple harmonic motion. Doubling $k$ doubles the restoring force at a fixed displacement, but increases that angular frequency only by a factor $\sqrt{2}$.

A finite collection of disjoint splitting spheres of a knot encodes a connected sum of knots. Cut along every sphere and fill each spherical boundary with a three-ball containing a straight arc joining its two marked endpoints. The resulting oriented knots are the factors. The system is complete when its nontrivial factors are prime knots.

A vector-spinor describes a spin-three-halves field after its lower-spin components are removed by constraints and, in the massless theory, gauge equivalence. The massless equation is invariant under ${\psi }_{\mu }\mapsto {\psi }_{\mu }+{\partial }_{\mu }\eta$. Gamma-trace gauge and the field equation give $\gamma \cdot \psi =\partial \cdot \psi =/\partial {\psi }_{\mu }=0$. Only helicities $\pm 3/2$ remain. A four-dimensional Majorana field has two physical polarizations; a complex field also has independent antiparticle modes. The gravitino is the supergravity realization of this field.

After complexification, pair the $D=2n$ Clifford algebra generators into $n$ fermionic creation and annihilation operators. Their occupation basis has $2^n$ states, giving the irreducible complex Dirac module. The chirality operator separates its even and odd occupation subspaces, each with $2^{n-1}$ states. Majorana reality conditions concern real dimensions and depend on spacetime signature; they must not be imposed in every even dimension indiscriminately.

Define ${\sigma }^{\mu \nu }=\frac{i}{2}[{\gamma }^{\mu },{\gamma }^{\nu }]$ using the gamma matrix Clifford algebra. Moving ${\gamma }^{\rho }$ through the two factors with $\{{\gamma }^{\mu },{\gamma }^{\nu }\}=2g^{\mu \nu }$ proves the displayed operator commutator. For real antisymmetric ${\omega }_{\mu \nu }$ and $S=1-\frac{i}{4}{\sigma }^{\mu \nu }{\omega }_{\mu \nu }$, it gives $S^{-1}{\gamma }^{\rho }S={\gamma }^{\rho }+{\omega }^{\rho }{}_{\nu }{\gamma }^{\nu }+O({\omega }^2)$. This is the infinitesimal Lorentz covariance identity required by the Dirac equation.

A chosen spin structure on a spin manifold defines the complex spinor bundle associated to the spin representation. In dimension $2m$ its vector bundle rank is $2^m$. Its chirality matrix is $\Gamma =i^{m}c(e^1)\cdots c(e^{2m})$ in the negative Clifford multiplication convention. It satisfies ${\Gamma }^2=1$ and anticommutes with each $c(e^i)$, giving $S=S^{+}\oplus S^{-}$ and an odd Dirac operator. In odd dimension there is no such canonical chiral splitting of the irreducible spinor bundle.

Lift the Levi-Civita connection to the spinor bundle using the spin representation of the Lorentz algebra. Under a local Lorentz transformation, its matrix ${\Omega }_{\mu }=\frac{1}{4}{\omega }_{\mu AB}{\gamma }^{AB}$ obeys ${\Omega }_{\mu }^{\prime }=S{\Omega }_{\mu }{S}^{-1}-({\partial }_{\mu }S)S^{-1}$, so ${\nabla }_{\mu }^{\prime }{\psi }^{\prime }=S{\nabla }_{\mu }\psi$. The Clifford algebra identity $[{\gamma }^C,{\gamma }^{AB}]=2({\eta }^{CA}{\gamma }^B-{\eta }^{CB}{\gamma }^A)$ fixes the coefficient. The tetrad postulate then gives ${\partial }_{\mu }{\gamma }^{\nu }+{\Gamma }_{\mu \rho }^{\nu }{\gamma }^{\rho }+[{\Omega }_{\mu },{\gamma }^{\nu }]=0$, establishing compatibility with curved Clifford multiplication.

The tetrad postulate expresses compatibility of the spacetime and Lorentz-frame connections on a vierbein. For the inverse coframe $e_{\nu }{}^b$, solving gives ${\omega }_a{}^{\mu }{}_{\nu }=e_{\nu }{}^b({\Gamma }^c{}_{ab}{e}^{\mu }{}_c-{\partial }_a{e}^{\mu }{}_b)$. Metric compatibility makes the lowered connection antisymmetric in its Lorentz indices. Lifting this connection through the Spinor representation of the Lorentz group defines the spinor covariant derivative.

For $g_{ab}={\Omega }^2{\eta }_{ab}$, use the vierbein $e^{\mu }{}_a=\Omega {\delta }^{\mu }{}_a$ and constant flat gamma matrices. The tetrad postulate and ${\Gamma }^c{}_{ab}={\delta }_a^c{\partial }_b\log \Omega +{\delta }_b^c{\partial }_a\log \Omega -{\eta }_{ab}{\eta }^{cd}{\partial }_d\log \Omega$ give the displayed lowered spin connection. With $L={\hat{\gamma }}^c{\partial }_c\log \Omega$, its spinor action is ${\nabla }_a={\partial }_a+[{\hat{\gamma }}_a,L]/4$. The Lorentz index lowering matters in indefinite signature.