A presymplectic form is a closed two-form, commonly assumed to have constant rank, that need not be nondegenerate. A symplectic form is its nondegenerate special case. Its kernel distribution is integrable: for kernel fields $X,Y$, the identity $d\omega =0$ gives ${\iota }_{[X,Y]}\omega =0$. If the characteristic leaf quotient is smooth and the form descends, that quotient has a symplectic form. A regular Hamiltonian energy hypersurface carries such a form with kernel spanned by its Hamiltonian vector field.

A real symmetric matrix is a Hermitian matrix, so $u^{\ast }Au$ is real for every complex vector $u$. If $u$ is an eigenvector, its eigenvalue is $(u^{\ast }Au)/(u^{\ast }u)$ and is real. Then $u^{\ast }Av=(Au{)}^{\ast }v$ gives $(\mu -\lambda )u^{\ast }v=0$. Reality is used in changing conjugate transpose to transpose; complex symmetry alone does not imply real eigenvalues.

Two real symmetric matrices are coaxial when they share an orthonormal eigenbasis. Equivalently they commute. Degenerate eigenspaces can have several choices of shared axes.

A real symmetric matrix is positive definite when its quadratic form is positive on every nonzero vector. By the spectral theorem, this is equivalent to all its eigenvalues being positive. It has a unique symmetric positive-definite square root.

Fix $v\ne 0$, put $s=v^{T}v$, $t=v^{T}Tv$, and $P=I-v{v}^T/s$. Any real symmetric matrix on three-dimensional Euclidean space has a unique decomposition with $C^{T}v=0$, $Dv=0$ and $\mathrm{tr}D=0$:The transverse restriction is a symmetric two-dimensional matrix, whose traceless matrix part has dimension two. Together the two scalars, two components of $C$ and two components of $D$ give the six parameters of $T$.

The displayed nonzero matrix is symmetric under transpose but not Hermitian. It is nilpotent, so all its eigenvalues are zero and it cannot be diagonalizable. Thus real-symmetric spectral conclusions require reality or a Hermitian hypothesis; complex transpose symmetry alone is insufficient.

Use the sequential convention ${\phi }_{;lmn}={\nabla }_n{\nabla }_m{\nabla }_l\phi$ and define $R$ by $X^a{}_{;mn}-X^a{}_{;nm}=R^a{}_{bmn}{X}^b$. The symmetric Hessian of a scalar field gives symmetry in $l,m$, but the curvature commutator on a covariant tensor gives ${\phi }_{;l[mn]}=-R^p{}_{lmn}{\phi }_{;p}/2$. Averaging the three distinct permutations yields ${\phi }_{;(lm)n}={\phi }_{;(lmn)}-(R^p{}_{lmn}+R^p{}_{mln}){\phi }_{;p}/3$. Thus a scalar's third covariant derivative is not generally totally symmetric.

The coefficient of $m_{\mu }$ in $f_{\lambda }$ counts distinct rearrangements of the parts of $\lambda$ whose prefix-sum set contains the prefix sums of $\mu$. Indeed, Hall inner product of symmetric functions duality between $m_{\lambda },h_{\lambda }$ turns this coefficient into $(-1{)}^{|\lambda |-\ell (\lambda )}$ times the coefficient of $h_{\lambda }$ in $e_{\mu }$. Expanding $E(t)=H(-t{)}^{-1}$ expresses each $e_{{\mu }_j}$ as a signed sum of compositions of ${\mu }_j$. Concatenating these compositions gives precisely the counted rearrangements, and every sign is $(-1{)}^{|\lambda |-\ell (\lambda )}$.

A subshift of finite type is a closed subset of a finite-alphabet full shift defined by finitely many forbidden finite words, with the restricted left shift. After replacing symbols by sufficiently long blocks, its constraints can be described by a zero-one symbolic transition matrix. In this presentation, membership means that every consecutive pair follows an allowed transition. The resulting sequence space is a compact metric space and the restricted left shift is a homeomorphism.

A sweat gland is a skin gland delivering secretion to the surface or a related follicular route. Eccrine glands are important in human evaporative cooling. Gland activation, fluid transport and environmental evaporation are separate determinants of the cooling achieved.

Suppose an unobserved class has probabilities $\pi$ and $1-\pi$, with hazard functions $q$ and $q+r$, and set $Q(t)={\int }_0^{t}q$, $R(t)={\int }_0^{t}r$. For an independently right-censored observation $(x,v)$, its survival-parameter likelihood contribution isThis sums the two class-specific likelihoods before taking a logarithm. All hazards must be nonnegative. A common parameter-free censoring mechanism factors out; class-specific censoring instead alters the mixture weights and cannot silently be discarded.

// Target: probability-and-statistics.bigb

Airy wave theory linearizes the motion of small-amplitude surface gravity waves in an inviscid, incompressible, irrotational fluid. At depth $h$, its dispersion relation is ${\omega }^2=gk\tanh (kh)$; deep water is the limit $kh\to \infty$.

The excess depth-integrated, time-averaged momentum flux of a surface gravity wave is its radiation stress. In deep water $c_g/c_p=1/2$, so $S_{xx}=\mathcal{E}/2={\rho }_{w}g{a}^2/4$. The force per transverse width on a reflecting object is the incident plus reflected minus transmitted radiation stress. Reflection increases force because the reflected wave carries momentum in the opposite direction.

For depth $h=\alpha x^p$ with $p>0$, stationary surface gravity waves conserve frequency $\omega$ and alongshore wavenumber $K$. Near shore their dispersion becomes ${\omega }^2\sim g{\kappa }^{2}h$, so $\kappa \sim \omega x^{-p/2}/\sqrt{g\alpha }$. The shoreward ray has $y^{\prime }\sim -K\sqrt{g\alpha }{x}^{p/2}/\omega$, giving the displayed integrated scaling. Rays approach normally, while equal-phase crests approach parallel to the shore and their shore-normal spacing shrinks as $x^{p/2}$. These are asymptotics within the ray approximation; for $p<2$, its slow-variation assumption eventually fails arbitrarily close to the endpoint.

For a tank with side lengths $a,b$, depth $h$, impermeable walls and negligible surface tension, the small-amplitude surface gravity wave normal modes have horizontal factors $\cos (m\pi x/a)\cos (n\pi y/b)$ and $k_{mn}^2=(m\pi /a{)}^2+(n\pi /b{)}^2$. The velocity potential has vertical factor $\cosh (k_{mn}(z+h))$, satisfying the bottom Neumann boundary condition. Combining the linearized free-surface boundary conditions gives ${\omega }_{mn}^2=g{k}_{mn}\tanh (k_{mn}h)$. The uniform $m=n=0$ surface elevation is excluded when the total water volume is fixed. Taking one horizontal index zero gives the two-dimensional tank modes.

For $k_{mn}h\ll 1$, the shallow-water approximation gives ${\omega }_{mn}\sim \sqrt{gh}{k}_{mn}$; for $k_{mn}h\gg 1$, the deep-water gravity wave relation ${\omega }_{mn}^2\sim g{k}_{mn}$ follows. An oscillating-wall forcing of a rectangular tank couples to these same normal modes and becomes resonant at their natural frequencies.

A surface gravity wave breaks when its smooth free-surface motion becomes unstable and overturns or forms a strongly dissipative front. In the nondispersive shallow-water approximation, intersecting compressive characteristic curves signal failure of a smooth simple wave; a hydraulic bore replaces it at the integral-model level. Dispersion can instead produce an oscillatory bore, while physical breaking involves turbulence and energy loss beyond the inviscid equations.

An optically thin spherical source with volume emissivity $j(r)=j_0{r}^{-p}$ has surface brightnessSubstitute $z=Ru$ in the line-of-sight integral and evaluate ${\int }_{-\infty }^{\infty }(1+u^2{)}^{-p/2}du$ using the beta function. The condition $p>1$ is convergence at large distance. A core or finite outer boundary changes the projection near that boundary; the stated scaling applies between those scales.

A Sérsic profile models projected galactic light, with index $n$ controlling curvature and $b_n$ chosen so that $R_e$ encloses half the luminosity. Its logarithmic slope is $d\ln I/d\ln R=-(b_n/n)(R/R_e{)}^{1/n}$. The $n=1$ case is exponential; $n=4$ gives the traditional de Vaucouleurs form. Unlike a fixed power law, its slope steepens outward.

In light-cone coordinates $x^{\pm }$ on two-dimensional Minkowski spacetime, add two real odd Grassmann variables ${\theta }^{\pm }$. With left Grassmann derivatives, the supercharges and supersymmetric covariant derivatives can be represented asThe identity $\{{\partial }_{\theta },\theta \}=1$ gives $Q_{\pm }^2=i{\partial }_{\pm }$, $D_{\pm }^2=-i{\partial }_{\pm }$, $\{Q_{+},Q_{-}\}=\{D_{+},D_{-}\}=0$, and $\{Q_s,D_t\}=0$ for every $s,t$. A Lorentz boost acts as $x^{\pm }\mapsto e^{\pm \omega }{x}^{\pm }$, ${\theta }^{\pm }\mapsto e^{\pm \omega /2}{\theta }^{\pm }$. Thus $D_{\pm }$ have boost weights $\mp 1/2$, and $D_{-}{D}_{+}$ is a Lorentz scalar. Since it commutes with both supercharges, an equation $i{D}_{-}{D}_{+}\Phi =W(\Phi )$ for an even scalar superfield is Lorentz invariant and supersymmetry covariant.

A local fermionic gauge symmetry of supersymmetric brane actions. Since the kappa symmetry projector has half rank, the symmetry removes half the embedding fermions. The remaining physical fermions pair with the bosonic worldvolume degrees of freedom.