A parametric surface is represented by a map $(u,v)\mapsto P(u,v)$. A regular patch has $P_u\times P_v\ne 0$; this cross product supplies its normal vector.

// Target: analysis.bigb

A parallel surface is a constant-distance normal displacement $P_d=P+dn$ of a regular surface with unit normal vector $n$. With shape operator $W=-Dn$, its differential is $(I-dW)DP$; it can become singular where $1-d{\kappa }_i=0$ for a principal curvature ${\kappa }_i$.

// Target: geometry-and-topology.bigb

A smooth embedded surface in ${\mathbb{R}}^3$ is a two-dimensional smooth manifold locally represented by an injective regular parametrized surface $\sigma :U\subset {\mathbb{R}}^2\to {\mathbb{R}}^3$, with ${\sigma }_u\times {\sigma }_v\ne 0$. The first fundamental form measures lengths and angles, and a choice of unit normal determines the second fundamental form, which measures bending. A surface with boundary additionally uses local half-plane charts along its boundary.

An Anosov flow is a nonsingular smooth flow on a compact smooth manifold with a continuous derivative-invariant splittingHere $F$ is the generating vector field, the flow direction is one-dimensional, and in the usual nontrivial convention both $E^s$ and $E^u$ have positive dimension. Constants $C,\lambda >0$ must work uniformly over all points, all $t\ge 0$ and the corresponding tangent vectors:The stable bundle of an Anosov flow contracts forward; the unstable bundle of an Anosov flow contracts backward. The neutral direction along $F$ is essential: changing the starting point slightly along an orbit mainly shifts its clock, so that direction cannot be included in either uniform contraction estimate.

A suspension flow of the cat map gives a three-dimensional example. A positive time change of a smooth flow preserves the Anosov property on a compact manifold, although its stable and unstable bundles can tilt along the flow direction. These are uniform structural conditions, stronger than a sign observed in one finite-time Lyapunov exponent calculation.

Write $\rho =1/f$ and $t={\int }_0^s\rho ({\varphi }_{r}x)dr$. For an Anosov stable bundle, the new stable directions are $v+{\lambda }_s(x,v)F(x)$, where ${\lambda }_s=\rho (x{)}^{-1}{\int }_0^{\infty }d{\rho }_{{\varphi }_{r}x}(D{\varphi }_{r}v)dr$. Exponential contraction makes this integral uniformly convergent. Differentiating the clock equation shows that its flow-direction coefficient after time $t$ is $\rho ({\varphi }_{s}x{)}^{-1}{\int }_s^{\infty }d\rho (D{\varphi }_{r}v)dr$, which decays exponentially and has the same graph form at the new point. Negative-time integrals give the unstable graph. Compactness and positivity of $f$ compare old and new times uniformly, preserving the Anosov flow property.

A suspension flow turns a discrete-time map into continuous motion by moving along an extra time coordinate. For a diffeomorphism $f:M\to M$ and constant roof one, form the mapping torusThe flow moves vertically at unit speed; each crossing of the top applies $f$ and re-enters at height zero. If $M$ has dimension $d$, the suspension has dimension $d+1$.

Suspending a hyperbolic toral automorphism gives an Anosov flow. After $k$ roof crossings, its transverse derivative is $A^k$, so the base map's stable and unstable exponential bounds become the transverse flow bounds. A remaining fractional crossing has a uniformly bounded effect on a compact mapping torus. The vertical direction supplies the neutral flow direction. In particular, the two-dimensional cat map gives a three-dimensional suspension.

A constant roof also shows why this flow need not be mixing. The well-defined height function $H([x,s])=e^{2\pi is}$ obeys $H({\Phi }_t([x,s]))=e^{2\pi it}H([x,s])$. Under the product invariant probability measure its mean is zero, but its autocorrelation has modulus one for all $t$. Thus even a mixing base map can produce a suspension with persistent clock correlations.

An observable $h$ is a flow coboundary if it is the derivative of a function $u$ along a flow map. An integrated formulation isWhen $u$ is differentiable along the flow, this is $Fu=h$, where $F$ is the generating vector field. Spatial regularity must be specified separately: $u$ may be smooth or merely Hölder continuous while still being differentiable along every flow line.

The function $c(t,x)=u({\Phi }_{t}x)-u(x)$ is a cocycle over a dynamical system. Its identity follows by adding the two differences from $x$ to ${\Phi }_{t}x$ and from ${\Phi }_{t}x$ to ${\Phi }_{s+t}x$. Being a coboundary says that the accumulated observable can be recovered from endpoint values.

For a periodic orbit of period $T$, the endpoint values coincide, so its integral of $h$ is zero. This is the periodic orbit obstruction. If $u$ is bounded, then the time average of $h$ also vanishes:For a transitive Anosov flow, the Livšic theorem identifies when the periodic-orbit obstruction is sufficient. This is stronger than checking just one average or finitely many periodic trajectories.

A curve parameter labels the points visited by a parametric curve $\gamma (t)$. Choosing time as the parameter determines its velocity; an arc-length parametrization instead measures accumulated arc length. A regular monotone reparametrization changes the labels and speed while preserving the route and its arc length.

For CW pairs $(X,A)$ and $(Y,B)$, write their product pair asUse the compactly generated product, equivalently the weak CW complex topology on products of cells. For arbitrary infinite CW complexes this can be finer than the ordinary product topology. The ordinary product topology already agrees when one factor is locally compact, or when both factors have countably many cells; in particular there is no distinction for finite CW complexes.^[ref]

The quotient of this pair is $(X/A)\wedge (Y/B)$. Setwise, the collapsed subset is exactly the set of pairs with at least one coordinate in its collapsed subspace; the compatible quotient constructions give the homeomorphism in the compactly generated space convention. In a multiplicative generalized cohomology theory, external products of relative classes of degrees $k,m$ lie in degree $k+m$ for this pair. Pullback along a diagonal map gives the relative cup product.

On a six-point set $X$ and its six totals of synthemes $Y$, each duad determines a partition of $Y$ into three pairs according to their shared synthemes. Include both whole halves, the 45 blocks $D\cup (Y\setminus P)$ for these duad-pair incidences, and their complements. For each partition $X=A\bigsqcup A^c$ into triples, cross synthemes give two triangular components on $Y$; include the four unions of a part of $X$ with a component. These 132 blocks form the small Witt design.

For the height profile $h(r)=r^{-2}-r^{-1}$, set $A=L^2+2g$ and use the planar small-slope model. Its effective potential per unit mass is $V_{\mathrm{eff}}=A/(2r^2)-g/r$. Release with negligible radial speed at $r_0$ gives $\mathcal{E}=A/(2r_0^2)-g/r_0$ and the displayed radial-speed law. A bounded trajectory requires $\mathcal{E}<0$, equivalently $r_0>A/(2g)$. The two positive turning radii are $r_0$ and $A{r}_0/(2g{r}_0-A)$; they coincide at the circular solution $r_0=A/g$. Zero energy is marginal escape, not bounded motion.

Along cosmological horizon exit $k\propto aH$, differentiation gives $d\log k/d\log a=1-{ϵ}_H$, where ${ϵ}_H=-\dot{H}/H^2$. The chain rule gives the first expression. In reduced Planck units, the slow-roll equations $3H\dot{\varphi }\simeq -V^{\prime }$ and $3H^2\simeq V$ give the second expression to leading order. Applied to a quantity already of slow-roll order, the omitted factor changes the answer only at second order.

With approximately constant positive $H$ and potential slope $V^{\prime }$, a homogeneous scalar field initially at rest solves $\ddot{\varphi }+3H\dot{\varphi }=-V^{\prime }$ with the displayed velocity. The transient decays on time $1/(3H)$, leaving the slow-roll approximation $3H\dot{\varphi }\simeq -V^{\prime }$. The fractional potential change over a Hubble time is of order $M_{\mathrm{Pl}}^2(V^{\prime }/V{)}^2$. Sustained slow roll normally uses both a small slope parameter and a small absolute curvature parameter $|M_{\mathrm{Pl}}^2{V}^{\prime \prime }/V|$. Local derivative bounds must hold over the traversed field interval; initial small kinetic energy alone is not a global inflation-duration theorem.

Now both plates at $z=0$ and $z=H$ are stationary and both obey the Navier slip boundary condition with the same slip length $b$. Drive steady flow of a Newtonian fluid in incompressible flow by the constant pressure gradient $G=-dp/dx>0$, with constant dynamic viscosity $\mu >0$ and no other streamwise body force. The planar Poiseuille flow profile and its volumetric flow rate per unit width areThe full volumetric flow rate for channel width $W$ is $Q=Wq$ when side-wall effects are negligible. Thus $q$ has units ${\mathrm{m}}^2{\mathrm{s}}^{-1}$, while $Q$ has units ${\mathrm{m}}^3{\mathrm{s}}^{-1}$. Denote the value at $b=0$ by $q_0=G{H}^3/(12\mu )$.

The two wall checks expose the normal signs:Both Navier slip boundary conditions therefore hold exactly. The two walls exert backward tangential tractions of magnitude $GH/2$ on the fluid. Increasing $b$ at fixed $G$ adds a uniform velocity offset, leaving the velocity gradient and wall shear stress unchanged. This differs from Couette flow with a slipping lower wall, where upper-wall velocity is fixed and shear stress decreases.

For $H=10\mu \mathrm{m}$, $b=2\mu \mathrm{m}$, $G=10^3\mathrm{Pa}{\mathrm{m}}^{-1}$ and $\mu =10^{-3}\mathrm{Pa}\mathrm{s}$, the wall velocity is $10\mu \mathrm{m}{\mathrm{s}}^{-1}$, the centre velocity is $22.5\mu \mathrm{m}{\mathrm{s}}^{-1}$, and $q=1.83\times 10^{-10}{\mathrm{m}}^2{\mathrm{s}}^{-1}$. The enhancement is $q/q_0=2.2$. Equivalently, a prescribed volumetric flow rate needs only $1/2.2$ of the original pressure gradient. This makes slip length useful for estimating pumping requirements in small channels.

At fixed $H$, $G>0$ and $\mu$, $b\to 0$ recovers ordinary planar Poiseuille flow. As $b\to \infty$, the velocity and $q$ grow without bound in this model, although the varying part of the profile stays the same. At exactly zero tangential wall traction, no steady solution can balance this nonzero pressure gradient: $u^{\prime }(0)=u^{\prime }(H)=0$ conflicts with $\mu [u^{\prime }(H)-u^{\prime }(0)]=-GH$. Unlimited enhancement is consequently not a prediction for a real channel; finite wall friction, finite driving capacity and the validity of the assumed steady flow must be assessed. At fixed finite $q$ instead, $G\to 0$ and the profile approaches uniform velocity $q/H$.

A short derivation integrates the reduced Navier-Stokes equation $\mu u^{\prime \prime }=-G$ twice. Equal slip lengths and the opposite inward unit normals give $u=G[z(H-z)+bH]/(2\mu )$. Its integral over the gap supplies the enhancement factor $1+6b/H$.

Consider steady flow of a Newtonian fluid in incompressible flow with constant dynamic viscosity $\mu >0$ between parallel plates at $z=0$ and $z=H$. The bottom plate is stationary and obeys the Navier slip boundary condition with slip length $b$. The top plate moves at velocity $U>0$ and obeys the no-slip boundary condition. There is no streamwise pressure gradient or body force. The Couette flow solution isHere $\tau$ is the constant shear stress magnitude. The lower wall's Navier slip boundary condition holds exactly because $b{u}^{\prime }(0)=bU/(H+b)=u(0)$. At the top, $u(H)=U$ is exactly the prescribed no-slip boundary condition; no finite upper-wall slip length is imposed in this example.

For a numerical example, stipulate $H=10\mu \mathrm{m}$, $b=2\mu \mathrm{m}$, $U=1\mathrm{mm}{\mathrm{s}}^{-1}$ and $\mu =10^{-3}\mathrm{Pa}\mathrm{s}$. The bottom velocity is $0.167\mathrm{mm}{\mathrm{s}}^{-1}$ and the shear stress is $0.0833\mathrm{Pa}$, compared with $0.100\mathrm{Pa}$ when both plates obey the no-slip boundary condition. The extrapolated profile reaches zero at $z=-2\mu \mathrm{m}$.

For fixed $H$, $U$ and $\mu$, $b\to 0$ recovers $u=Uz/H$. As $b\to \infty$, $u\to U$ throughout the gap and $\tau \to 0$: the moving upper wall selects the limiting uniform velocity, while the lower wall approaches a stress-free boundary condition. The dynamic viscosity stays positive; the disappearing shear stress comes from the disappearing velocity gradient.

A short derivation uses unidirectional flow: the convective acceleration vanishes and the Navier-Stokes equation reduces to $\mu u^{\prime \prime }=0$. Write $u=Az+B$. The bottom condition gives $B=bA$ and the top condition gives $A(H+b)=U$.

For a spatially dilated Skyrme model field $U_L(x)=U(x/L)$, the quadratic and quartic derivative energies scale as shown. A static stationary field must satisfy $(d-2)E_2+(d-4)E_4=0$. In three spatial dimensions this permits $E_2=E_4$ and a positive second variation along scale. In two dimensions it requires $E_4=0$, and in four or more it forces a constant finite-energy smooth field. In one dimension the commutator term vanishes identically. Derrick scaling tests a necessary variational condition, not existence or stability under all deformations.

Let $T$ be a minimal homeomorphism of a compact metric space $X$, and let $\rho :X\to \mathbb{R}/\mathbb{Z}$ be continuous. The circle skew productis a minimal dynamical system precisely when there is no continuous circle-valued function $f$ satisfyingfor any nonzero integer $m$.

A solution gives an explicit obstruction: $e^{2\pi imy}/f(x)$ is a nonconstant continuous function invariant under $S$. Its level sets are proper closed invariant sets, so the extension is not minimal.

Conversely, take a minimal subsystem of a nonminimal extension. Its vertical translation stabilizer is a proper closed subgroup of the circle, and its fibers are cosets of that subgroup. A nontrivial circle character trivial on the subgroup descends to a continuous circle-valued function of the base, giving the displayed forbidden equation. Compactness and the isometric circle action supply this coset description; arbitrary nonisometric fiber dynamics need not have it.

For a base consisting of one point and constant $\rho =\alpha$, the equation reduces to $e^{2\pi im\alpha }=1$. Its absence for every nonzero $m$ says exactly that $\alpha$ is irrational, recovering minimality of an irrational rotation of the circle.

For two otherwise symmetric SIS models with recovery rate $\gamma$, primary transmission $\beta$ and secondary susceptibility multiplier $q$, split hosts into uninfected, singly infected and doubly infected classes. The displayed conditions give stable disease-free and joint endemic states, with an intermediate saddle: a strong Allee effect. The endemic susceptible fraction solves $(q-1)S^2-qS+{\mathcal{R}}_0^{-2}=0$. The smaller root is the stable high-prevalence state. Coinfected hosts recover each infection independently, so recovery from coinfection leads to a single-infection class rather than directly to complete susceptibility.

For $\dot{i}=\beta i(1-i)-\gamma i$, a positive endemic equilibrium requires $R_0=\beta /\gamma >1$ and gives susceptible fraction $s_{\ast }=\gamma /\beta$. Below threshold the disease-free susceptible fraction is one. The reciprocal relation is a property of this homogeneous scalar SIS model, not a universal identity for heterogeneous populations.

For high-risk group fraction $p$, fixed total contact rates and reciprocal cross-group contacts, let $C=Bp/(1-p)$. The displayed SIS model describes within-group infectious fractions. In fractions the transmission matrix is $M=\left(\begin{array}{cc}A& B\\ C& D-C\end{array}\right)$; in infected-person counts it is $\mathrm{diag}(p,1-p)M\mathrm{diag}(p,1-p{)}^{-1}$. A common recovery rate gives basic reproduction number $\rho (M)/\gamma$. The mean population susceptible fraction does not generally equal its reciprocal.