D'Alembert's paradox

thumb|Jean le Rond d'Alembert (1717-1783)

right|thumb|From [[experiments it is known that there is always – except in case of superfluidity – a drag force for a body placed in a steady fluid onflow. The figure shows the drag coefficient Cd for a sphere as a function of Reynolds number Re, as obtained from laboratory experiments. The dark line is for a sphere with a smooth surface, while the lighter line is for the case of a rough surface. The numbers along the line indicate several flow regimes and associated changes in the drag coefficient:

•2: attached flow (Stokes flow) and steady separated flow,

•3: separated unsteady flow, having a laminar flow boundary layer upstream of the separation, and producing a vortex street,

•4: separated unsteady flow with a laminar boundary layer at the upstream side, before flow separation, with downstream of the sphere a chaotic turbulent wake,

•5: post-critical separated flow, with a turbulent boundary layer.]]

In fluid dynamics, d'Alembert's paradox (or the hydrodynamic paradox) is a paradox discovered in 1752 by French mathematician Jean le Rond d'Alembert. D'Alembert proved that – for incompressible and inviscid potential flow – the drag force is zero on a body moving with constant velocity relative to (and simultaneously through) the fluid. Zero drag is in direct contradiction to the observation of substantial drag on bodies moving relative to and at the same time through a fluid, such as air and water; especially at high velocities corresponding with high Reynolds numbers. It is a particular example of the reversibility paradox.

D’Alembert, working on a 1749 Prize Problem of the Berlin Academy on flow drag, concluded:

A physical paradox indicates flaws in the theory.

Fluid mechanics was thus discredited by engineers from the start, which resulted in an unfortunate split – between the field of hydraulics, observing phenomena which could not be explained, and theoretical fluid mechanics explaining phenomena which could not be observed – in the words of the Chemistry Nobel Laureate Sir Cyril Hinshelwood.

According to scientific consensus, the occurrence of the paradox is due to the neglected effects of viscosity. In conjunction with scientific experiments, there were huge advances in the theory of viscous fluid friction during the 19th century. With respect to the paradox, this culminated in the discovery and description of thin boundary layers by Ludwig Prandtl in 1904. Even at very high Reynolds numbers, the thin boundary layers remain as a result of viscous forces. These viscous forces cause friction drag on streamlined objects, and for bluff bodies the additional result is flow separation and a low-pressure wake behind the object, leading to form drag.

The general view in the fluid mechanics community is that, from a practical point of view, the paradox is solved along the lines suggested by Prandtl. A formal mathematical proof is lacking, and difficult to provide, as in so many other fluid-flow problems involving the Navier–Stokes equations (which are used to describe viscous flow).

Viscous friction: Saint-Venant, Navier and Stokes

First steps towards solving the paradox were made by Adhémar Barré de Saint-Venant, who modelled viscous fluid friction. Saint-Venant states in 1847:

Soon after, in 1851, George Gabriel Stokes calculated the drag on a sphere in Stokes flow, known as Stokes' law. Stokes flow is the low Reynolds-number limit of the Navier–Stokes equations describing the motion of a viscous liquid.

However, when the flow problem is put into a non-dimensional form, the viscous Navier–Stokes equations converge for increasing Reynolds numbers towards the inviscid Euler equations, suggesting that the flow should converge towards the inviscid solutions of potential flow theory – having the zero drag of the d'Alembert paradox. Of this, there is no evidence found in experimental measurements of drag and flow visualisations. In the second half of the 19th century this again raised questions concerning the applicability of fluid mechanics.

Inviscid separated flow: Kirchhoff and Rayleigh

thumb|right|300px|Steady and separated incompressible potential flow around a plate in two dimensions, with a constant pressure along the two free streamlines separating from the plate edges.

In the second half of the 19th century, focus shifted again towards using inviscid flow theory for the description of fluid drag—assuming that viscosity becomes less important at high Reynolds numbers. The model proposed by Kirchhoff

and Rayleigh

was based on the free-streamline theory of Helmholtz and consists of a steady wake behind the body. Assumptions applied to the wake region include: flow velocities equal to the body velocity, and a constant pressure. This wake region is separated from the potential flow outside the body and wake by vortex sheets with discontinuous jumps in the tangential velocity across the interface.

In order to have a non-zero drag on the body, the wake region must extend to infinity. This condition is indeed fulfilled for the Kirchhoff flow perpendicular to a plate. The theory correctly states the drag force to be proportional to the square of the velocity.

In first instance, the theory could only be applied to flows separating at sharp edges. Later, in 1907, it was extended by Levi-Civita to flows separating from a smooth curved boundary.

It was readily known that such steady flows are not stable, since the vortex sheets develop so-called Kelvin–Helmholtz instabilities.

Moreover, the observed pressure differences between front and back of the plate, and resulting drag forces, are much larger than predicted: for a flat plate perpendicular to the flow the predicted drag coefficient is CD=0.88, while in experiments CD=2.0 is found. This is mainly due to suction at the wake side of the plate, induced by the unsteady flow in the real wake (as opposed to the theory which assumes a constant flow velocity equal to the plate's velocity).

So, this theory is found to be unsatisfactory as an explanation of drag on a body moving through a fluid. Although it can be applied to so-called cavity flows where, instead of a wake filled with fluid, a vacuum cavity is assumed to exist behind the body.

Thin boundary layers: Prandtl

thumb|right|300px|Pressure distribution for the flow around a circular cylinder. The dashed blue line is the pressure distribution according to [[potential flow theory, resulting in d'Alembert's paradox. The solid blue line is the mean pressure distribution as found in experiments at high Reynolds numbers. The pressure is the radial distance from the cylinder surface; a positive pressure (overpressure) is inside the cylinder, towards the centre, while a negative pressure (underpressure) is drawn outside the cylinder.]]

The German physicist Ludwig Prandtl suggested in 1904 that the effects of a thin viscous boundary layer possibly could be the source of substantial drag. Prandtl put forward the idea that, at high velocities and high Reynolds numbers, a no-slip boundary condition causes a strong variation of the flow speeds over a thin layer near the wall of the body. This leads to the generation of vorticity and viscous dissipation of kinetic energy in the boundary layer. The energy dissipation, which is lacking in the inviscid theories, results for bluff bodies in separation of the flow. The low pressure in the wake region causes form drag, and this can be larger than the friction drag due to the viscous shear stress at the wall.

Open questions

To verify, as Prandtl suggested, that a vanishingly small cause (vanishingly small viscosity for increasing Reynolds number) has a large effect – substantial drag —

may be very difficult.

The mathematician Garrett Birkhoff in the opening chapter of his book Hydrodynamics from 1950, addresses a number of paradoxes of fluid mechanics (including d'Alembert's paradox) and expresses a clear doubt in their official resolutions:

:"Moreover, I think that to attribute them all to the neglect of viscosity is an unwarranted oversimplification The root lies deeper, in lack of precisely that deductive rigor whose importance is so commonly minimized by physicists and engineers."

In particular, on d'Alembert's paradox, he considers another possible route to the creation of drag: instability of the potential flow solutions to the Euler equations. Birkhoff states:

:"In any case, the preceding paragraphs make it clear that the theory of non-viscous flows is incomplete. Indeed, the reasoning leading to the concept of a "steady flow" is inconclusive; there is no rigorous justification for the elimination of time as an independent variable. Thus though Dirichlet flows (potential solutions) and other steady flows are mathematically possible, there is no reason to suppose that any steady flow is stable."

In his 1951 review of Birkhoff's book, the mathematician James J. Stoker sharply criticizes the first chapter of the book:

:"The reviewer found it difficult to understand for what class of readers the first chapter was written. For readers that are acquainted with hydrodynamics the majority of the cases cited as paradoxes belong either to the category of mistakes long since rectified, or in the category of discrepancies between theory and experiments the reasons for which are also well understood. On the other hand, the uninitiated would be very likely to get the wrong ideas about some of the important and useful achievements in hydrodynamics from reading this chapter."

In the second and revised edition of Birkhoff's Hydrodynamics in 1960, the above two statements no longer appear.

The importance and usefulness of the achievements, made on the subject of the d'Alembert paradox, are reviewed by Keith Stewartson thirty years later. His long 1981 survey article starts with: In the case of d'Alembert's paradox, the essential mechanism for its resolution was provided by Prandtl through the discovery and modelling of thin viscous boundary layers – which are non-vanishing at high Reynolds numbers.

An inviscid fluid is described by the Euler equations, which together with the other two conditions read

:<math> \begin{align}

& \mathbf{\nabla} \cdot \mathbf{u} = 0 && \text{(incompressibility)} \\

& \mathbf{\nabla}\times\mathbf{u}=0 && \text{(irrotational)} \\

& \frac{\partial}{\partial t} \mathbf{u} + \left(\mathbf{u} \cdot \mathbf{\nabla}\right) \mathbf{u} = - \frac{1}{\rho} \mathbf{\nabla} p && \text{(Euler equation)}

\end{align} </math>

where u denotes the flow velocity of the fluid, p the pressure, ρ the density, and ∇ is the gradient operator.

We have the second term in the Euler equation as:

:<math> \left(\mathbf{u} \cdot \mathbf{\nabla}\right) \mathbf{u} = \tfrac12 \mathbf{\nabla} \left(\mathbf{u} \cdot \mathbf{u}\right) - \mathbf{u} \times \mathbf{\nabla} \times \mathbf{u} = \tfrac12 \mathbf{\nabla} \left(\mathbf{u} \cdot \mathbf{u}\right) \qquad (1)</math>

where the first equality is a vector calculus identity and the second equality uses that the flow is irrotational. Furthermore, for every irrotational flow, there exists a velocity potential φ such that u = ∇φ. Substituting this all in the equation for momentum conservation yields

:<math> \mathbf{\nabla} \left( \frac{\partial\varphi}{\partial t} + \tfrac12 \mathbf{u} \cdot \mathbf{u} + \frac p\rho \right) = \mathbf{0}. </math>

Thus, the quantity between brackets must be constant (any t-dependence can be eliminated by redefining φ). Assuming that the fluid is at rest at infinity and that the pressure is defined to be zero there, this constant is zero, and thus

:<math> \frac{\partial\varphi}{\partial t} + \tfrac12 \mathbf{u} \cdot \mathbf{u} + \frac p\rho = 0, \qquad (2) </math>

which is the Bernoulli equation for unsteady potential flow.

Zero drag

Now, suppose that a body moves with constant velocity v through the fluid, which is at rest infinitely far away. Then the velocity field of the fluid has to follow the body, so it is of the form , where x is the spatial coordinate vector, and thus:

:<math> \frac{\partial \mathbf{u{\partial t} + \left( \mathbf{v} \cdot \boldsymbol{\nabla} \right) \mathbf{u} = \mathbf{0}. </math>

Since u = ∇φ, this can be integrated with respect to x:

:<math>\frac{\partial\varphi}{\partial t} = -\mathbf{v} \cdot \boldsymbol{\nabla} \varphi + R(t) = -\mathbf{v} \cdot \mathbf{u} + R(t). </math>

The force F that the fluid exerts on the body is given by the surface integral

:<math> \mathbf{F} = - \int_A p\, \mathbf{n}\; \mathrm{d} S </math>

where A denotes the body surface and n the normal vector on the body surface. But it follows from (2) that

:<math> p = - \rho \left( \frac{\partial\varphi}{\partial t} + \tfrac12 \mathbf{u} \cdot \mathbf{u} \right) = \rho \left( \mathbf{v} \cdot \mathbf{u} - \tfrac12 \mathbf{u} \cdot \mathbf{u} - R(t) \right), </math>

thus

:<math > \mathbf{F} = - \int_A p\, \mathbf{n}\; \mathrm{d} S = \rho \int_A \left(\tfrac12 \mathbf{u} \cdot \mathbf{u} - \mathbf{v} \cdot \mathbf{u}\right) \mathbf{n}\; \mathrm{d} S, </math>

with the contribution of R(t) to the integral being equal to zero.

At this point, it becomes more convenient to work in the vector components. The kth component of this equation reads

:<math > F_k = \rho \int_A \sum_i (\tfrac12 u_i^2 - u_i v_i) n_k \, \mathrm{d} S. \qquad (3) </math>

Let V be the volume occupied by the fluid. The divergence theorem says that

:<math> \frac12 \int_A \sum_i u_i^2 n_k \, \mathrm{d} S = - \frac12 \int_V \frac{\partial}{\partial x_k} \left( \sum_i u_i^2 \right) \,\mathrm{d} V. </math>

The right-hand side is an integral over an infinite volume, so this needs some justification, which can be provided by appealing to potential theory to show that the velocity u must fall off as r−3 – corresponding to a dipole potential field in case of a three-dimensional body of finite extent – where r is the distance to the centre of the body. The integrand in the volume integral can be rewritten as follows:

:<math > \frac12 \frac{\partial}{\partial x_k} \left( \sum_i u_i^2 \right) = \sum_i u_i \frac{\partial u_k}{\partial x_i} = \sum_i \frac{\partial(u_iu_k)}{\partial x_i} </math>

where first equality (1) and then the incompressibility of the flow are used. Substituting this back into the volume integral and another application of the divergence theorem again. This yields

:<math> - \frac12 \int_V \frac{\partial}{\partial x_k} \left( \sum_i u_i^2 \right) \,\mathrm{d} V = -\int_V \sum_i \frac{\partial(u_iu_k)}{\partial x_i} \,\mathrm{d} V = \int_A u_k \sum_i u_i n_i \,\mathrm{d} S.</math>

Substituting this in (3), we find that

:<math> F_k = \rho \int_A \sum_i (u_k u_i n_i - v_i u_i n_k) \, \mathrm{d} S. </math>

The fluid cannot penetrate the body and thus n · u = n · v on the body surface. So <math display="inline"> \sum_i n_i\, v_i = \sum_i n_i\, u_i</math> and

:<math > F_k = \rho \int_A \sum_i (u_k v_i n_i - v_i u_i n_k) \, \mathrm{d} S. </math>

Finally, the drag is the force in the direction in which the body moves, so

:<math > \mathbf v \cdot \mathbf F = \sum_k v_k F_k = 0. </math>

Hence the drag vanishes. This is d'Alembert's paradox.

Notes

References

Historical

External links

Potential Flow and d'Alembert's Paradox at MathPages